# Bohmian Mechanics

*First published Fri Oct 26, 2001; substantive revision Fri May 19, 2006*

Bohmian mechanics, which is also called the de Broglie-Bohm theory, the pilot-wave model, and the causal interpretation of quantum mechanics, is a version of quantum theory discovered by Louis de Broglie in 1927 and rediscovered by David Bohm in 1952. It is the simplest example of what is often called a hidden variables interpretation of quantum mechanics. In Bohmian mechanics a system of particles is described in part by its wave function, evolving, as usual, according to Schrödinger's equation. However, the wave function provides only a partial description of the system. This description is completed by the specification of the actual positions of the particles. The latter evolve according to the "guiding equation," which expresses the velocities of the particles in terms of the wave function. Thus, in Bohmian mechanics the configuration of a system of particles evolves via a deterministic motion choreographed by the wave function. In particular, when a particle is sent into a two-slit apparatus, the slit through which it passes and where it arrives on the photographic plate are completely determined by its initial position and wave function.

Bohmian mechanics inherits and makes explicit the nonlocality implicit in the notion, common to just about all formulations and interpretations of quantum theory, of a wave function on the configuration space of a many-particle system. It accounts for all of the phenomena governed by nonrelativistic quantum mechanics, from spectral lines and scattering theory to superconductivity, the quantum Hall effect and quantum computing. In particular, the usual measurement postulates of quantum theory, including collapse of the wave function and probabilities given by the absolute square of probability amplitudes, emerge from an analysis of the two equations of motion — Schrödinger's equation and the guiding equation - without the traditional invocation of a special, and somewhat obscure, status for observation.

- 1. The Completeness of the Quantum Mechanical Description
- 2. The Impossibility of Hidden Variables ... or the Inevitability of Nonlocality?
- 3. History
- 4. The Defining Equations of Bohmian Mechanics
- 5. The Quantum Potential
- 6. The Two-Slit Experiment
- 7. The Measurement Problem
- 8. The Collapse of the Wave Function
- 9. Quantum Randomness
- 10. Quantum Observables
- 11. Spin
- 12. Contextuality
- 13. Nonlocality
- 14. Lorentz Invariance
- 15. Objections
- Bibliography
- Other Internet Resources
- Related Entries

## 1. The Completeness of the Quantum Mechanical Description

Despite its extraordinary predictive successes, quantum mechanics has, since its inception some seventy years ago, been plagued by conceptual difficulties. The basic problem, plainly put, is this: It is not at all clear what quantum mechanics is about. What, in fact, does quantum mechanics describe?

It might seem, since it is widely agreed that any quantum mechanical system is completely described by its wave function, that quantum mechanics is fundamentally about the behavior of wave functions. Quite naturally, no physicist wanted this to be true more than did Erwin Schrödinger, the father of the wave function. Nonetheless, Schrödinger ultimately found this impossible to believe. His difficulty was not so much with the novelty of the wave function (Schrödinger 1935): "That it is an abstract, unintuitive mathematical construct is a scruple that almost always surfaces against new aids to thought and that carries no great message." Rather, it was that the "blurring" suggested by the spread out character of the wave function "affects macroscopically tangible and visible things, for which the term ‘blurring’ seems simply wrong."

For example, in the same paper Schrödinger noted that it may happen in radioactive decay that

the emerging particle is described ... as a spherical wave ... that impinges continuously on a surrounding luminescent screen over its full expanse. The screen however does not show a more or less constant uniform surface glow, but rather lights up atoneinstant atonespot ....

And he observed that one can easily arrange, for example by including a cat in the system, "quite ridiculous cases" with

the ψ-function of the entire system having in it the living and the dead cat (pardon the expression) mixed or smeared out in equal parts.

It is thus because of the "measurement problem," of macroscopic superpositions, that Schrödinger found it difficult to regard the wave function as "representing reality." But then what does? With evident disapproval, Schrödinger describes how

the reigning doctrine rescues itself or us by having recourse to epistemology. We are told that no distinction is to be made between the state of a natural object and what I know about it, or perhaps better, what I can know about it if I go to some trouble. Actually — so they say — there is intrinsically only awareness, observation, measurement.

Many physicists pay lip service to the Copenhagen interpretation
— that quantum mechanics is fundamentally about observation or
results of measurement. But it is becoming increasingly difficult to
find any who, when pressed, will defend this interpretation. It seems
clear that quantum mechanics is fundamentally about atoms and
electrons, quarks and strings, not those particular macroscopic
regularities associated with what we call *measurements* of the
properties of these things. But if these entities are not to be somehow
identified with the wave function itself — and if talk of them is
not merely shorthand for elaborate statements about measurements
— then where are they to be found in the quantum description?

There is, perhaps, a very simple reason why there has been so much difficulty discerning in the quantum description the objects we believe quantum mechanics should be describing. Perhaps the quantum mechanical description is not the whole story, a possibility most prominently associated with Albert Einstein.

In 1935 Einstein, Boris Podolsky and Nathan Rosen argued for this possibility in the famous EPR paper (Einstein et al. 1935), which they concluded with the following:

While we have thus shown that the wave function does not provide a complete description of the physical reality, we left open the question of whether or not such a description exists. We believe, however, that such a theory is possible.

The argument given in the EPR paper for this conclusion invoked quantum correlations and an assumption of locality. (See the entry on quantum entanglement and information.)

Later, on the basis of more or less the same considerations as those of Schrödinger quoted above, Einstein again concluded that the wave function does not provide a complete description of individual systems, an idea he called "this most nearly obvious interpretation" (Einstein 1949, p. 672). In relation to a theory incorporating a more complete description, Einstein remarked that "the statistical quantum theory would ... take an approximately analogous position to the statistical mechanics within the framework of classical mechanics." It is perhaps worth noting here that Bohmian mechanics, as we shall see, exactly fits this description.

## 2. The Impossibility of Hidden Variables ... or the Inevitability of Nonlocality?

John von Neumann, one of the greatest mathematicians of the twentieth century, claimed to have mathematically proven that Einstein's dream, of a deterministic completion or reinterpretation of quantum theory, was mathematically impossible. He concluded that (von Neumann 1932, p. 325 of the English translation)

It is therefore not, as is often assumed, a question of a re-interpretation of quantum mechanics — the present system of quantum mechanics would have to be objectively false, in order that another description of the elementary processes than the statistical one be possible.

This claim of von Neumann was almost universally accepted among physicists and philosophers of science. For example, Max Born, who formulated the statistical interpretation of the wave function, assured us that (Born 1949, p. 109)

No concealed parameters can be introduced with the help of which the indeterministic description could be transformed into a deterministic one. Hence if a future theory should be deterministic, it cannot be a modification of the present one but must be essentially different.

Bohmian mechanics is, quite clearly, a counterexample to the claims
of von Neumann, so something has to be wrong with von Neumann's
argument. In fact, according to John Bell (Mermin 1993, p. 805), von
Neumann's assumptions (about the relationships among the values of
quantum observables that must be satisfied in a hidden-variables
theory) are so unreasonable that the "the proof of von Neumann is not
merely false but *foolish*!" Nonetheless, some physicists
continue to rely on von Neumann's proof, although in recent years it is
more common to find physicists citing the
Kochen-Specker Theorem
and, more
frequently, Bell's inequality as the basis of this refutation. We still
find, a quarter of a century after the rediscovery of Bohmian mechanics
in 1952, statements such as these (Wigner 1976):

The proof he [von Neumann] published ..., though it was made much more convincing later on by Kochen and Specker, still uses assumptions which, in my opinion, can quite reasonably be questioned. ... In my opinion, the most convincing argument against the theory of hidden variables was presented by J. S. Bell (1964).

Now there are many more statements of a similar character that could have been cited. This quotation owes its significance to the fact that Wigner was not only one of the leading physicists of his generation, but, unlike most of his contemporaries, he was also profoundly concerned with the conceptual foundations of quantum mechanics and wrote on the subject with great clarity and insight.

There was, however, one physicist who wrote on this subject with even greater clarity and insight than Wigner himself, namely the very J. S. Bell whom Wigner praises for demonstrating the impossibility of a deterministic completion of quantum theory such as Bohmian mechanics. Here's how Bell himself reacted to Bohm's discovery (Bell 1987, p. 160):

But in 1952 I saw the impossible done. It was in papers by David Bohm. Bohm showed explicitly how parameters could indeed be introduced, into nonrelativistic wave mechanics, with the help of which the indeterministic description could be transformed into a deterministic one. More importantly, in my opinion, the subjectivity of the orthodox version, the necessary reference to the ‘observer,’ could be eliminated. ...But why then had Born not told me of this ‘pilot wave’? If only to point out what was wrong with it? Why did von Neumann not consider it? More extraordinarily, why did people go on producing ‘‘impossibility’’ proofs, after 1952, and as recently as 1978? ... Why is the pilot wave picture ignored in text books? Should it not be taught, not as the only way, but as an antidote to the prevailing complacency? To show us that vagueness, subjectivity, and indeterminism, are not forced on us by experimental facts, but by deliberate theoretical choice?

Wigner to the contrary notwithstanding, Bell did not establish the impossibility of a deterministic reformulation of quantum theory, nor did he ever claim to have done so. On the contrary, over the course of the past several decades, until his untimely death in 1990, Bell was the prime proponent, for a good part of this period almost the sole proponent, of the very theory, Bohmian mechanics, that he is supposed to have demolished.

Bohmian mechanics is of course as much a counterexample to the Kochen-Specker argument for the impossibility of hidden variables as it is to the one of von Neumann. It is obviously a counterexample to any such argument. However reasonable the assumptions of such an argument, some of them must fail for Bohmian mechanics.

Wigner was quite right to suggest that the assumptions of Kochen and Specker are more convincing than those of von Neumann. They appear, in fact, to be quite reasonable indeed . However, they are not. The impression that they are arises from a pervasive error, a naive realism about operators, that will be discussed below in the sections on quantum observables, on spin, and on contextuality.

One of the achievements of John Bell was to replace the "arbitrary axioms" (Bell 1987, page 11) of Kochen-Specker and others by an assumption of locality, of no action-at-a-distance. It would be hard to argue against the reasonableness of such an assumption, even if one were so bold as to doubt its inevitability. Bell showed that any hidden-variables formulation of quantum mechanics must be nonlocal, as, indeed, Bohmian mechanics is. But he showed much much more.

In a celebrated paper published in 1964, Bell showed that quantum theory itself is irreducibly nonlocal. This fact about quantum mechanics, based as it is on a short and mathematically simple analysis, could have been recognized soon after the discovery of quantum theory in the 1920's. That this did not happen is no doubt due in part to the obscurity of orthodox quantum theory and to the ambiguity of its commitments. It was, in fact, his examination of Bohmian mechanics that led Bell to his nonlocality analysis. In the course of his investigation of Bohmian mechanics he observed that (Bell 1987, p. 11):

in this theory an explicit causal mechanism exists whereby the disposition of one piece of apparatus affects the results obtained with a distant piece.Bohm of course was well aware of these features of his scheme, and has given them much attention. However, it must be stressed that, to the present writer's knowledge, there is no

proofthatanyhidden variable account of quantum mechanicsmusthave this extraordinary character. It would therefore be interesting, perhaps, to pursue some further "impossibility proofs," replacing the arbitrary axioms objected to above by some condition of locality, or of separability of distant systems.

In a footnote, Bell added that "Since the completion of this paper such a proof has been found." This proof was published in his 1964 paper, "On the Einstein-Podolsky-Rosen Paradox," in which he derives Bell's inequality, the basis of his conclusion of quantum nonlocality. (For a discussion of how nonlocality emerges in Bohmian mechanics, see Section 13.)

It is worth stressing that Bell's analysis indeed shows that any account of quantum phenomena must be nonlocal, not just any hidden variables account. Bell showed that nonlocality is implied by the predictions of standard quantum theory itself. Thus if nature is governed by these predictions, then nature is nonlocal. [That nature is so governed, even in the crucial EPR-correlation experiments, has by now been established by a great many experiments, the most conclusive of which is perhaps that of Aspect (Aspect et al., 1982).]

Bell, too, stressed this point (by determinism Bell here means hidden variables):

It is important to note that to the limited degree to whichdeterminismplays a role in the EPR argument, it is not assumed butinferred. What is held sacred is the principle of ‘local causality’ — or ‘no action at a distance’...It is remarkably difficult to get this point across, that determinism is not a

presuppositionof the analysis. (Bell 1987, p. 143)Despite my insistence that the determinism was inferred rather than assumed, you might still suspect somehow that it is a preoccupation with determinism that creates the problem. Note well then that the following argument makes no mention whatever of determinism. ... Finally you might suspect that the very notion of particle, and particle orbit ... has somehow led us astray. ... So the following argument will not mention particles, nor indeed fields, nor any other particular picture of what goes on at the microscopic level. Nor will it involve any use of the words ‘quantum mechanical system’, which can have an unfortunate effect on the discussion. The difficulty is not created by any such picture or any such terminology. It is created by the predictions about the correlations in the visible outputs of certain conceivable experimental set-ups. (Bell 1987, p. 150)

The "problem" and "difficulty" to which Bell refers above is the conflict between the predictions of quantum theory and what can be inferred, call it C, from an assumption of locality in Bohm's version of the EPR argument, a conflict established by Bell's inequality. C happens to concern the existence of a certain kind of hidden variables, what might be called local hidden variables, but this fact is of little substantive importance. What is important is not so much the identity of C as the fact that C is incompatible with the predictions of quantum theory. The identity of C is, however, of great historical significance: It is responsible for the misconception that Bell proved that hidden variables are impossible, a belief until recently almost universally shared by physicists, as well as for the view, even now almost universally held, that what Bell's result does is to rule out local hidden variables, a view that is misleading.

Here again is Bell, expressing the logic of his *two-part*
demonstration of quantum nonlocality, the first part of which is Bohm's
version of the EPR argument:

Let me summarize once again the logic that leads to the impasse. The EPRB correlations are such that the result of the experiment on one side immediately foretells that on the other, whenever the analyzers happen to be parallel. If we do not accept the intervention on one side as a causal influence on the other, we seem obliged to admit that the results on both sides are determined in advance anyway, independently of the intervention on the other side, by signals from the source and by the local magnet setting. But this has implications for non-parallel settings which conflict with those of quantum mechanics. So wecannotdismiss intervention on one side as a causal influence on the other. (Bell 1987, p. 149)

## 3. History

The pilot-wave approach to quantum theory was initiated, even before
the discovery of quantum mechanics itself, by Einstein, who hoped that
interference phenomena involving particle-like photons could be
explained if the motion of the photons were somehow guided by the
electromagnetic field — which would thus play the role of what he
called a *Führungsfeld* or guiding field (Wigner 1976, p.
262). While the notion of the electromagnetic field as guiding field
turned out to be rather problematical, the possibility that for a
system of electrons the wave function might play this role, of guiding
field or pilot wave, was explored by Max Born in his early paper
founding quantum scattering theory (Born 1926) — a suggestion to
which Heisenberg was profoundly unsympathetic.

Not long after Schrödinger's discovery, in 1926, of wave mechanics, i.e., of Schrödinger's equation, Louis de Broglie in effect discovered Bohmian mechanics: In 1927, de Broglie found an equation of particle motion equivalent to the guiding equation for a scalar wave function (de Broglie 1928, p. 119), and he explained at the 1927 Solvay Congress how this motion could account for quantum interference phenomena. However, de Broglie responded poorly to an objection of Wolfgang Pauli (Pauli 1928) concerning inelastic scattering, no doubt making a rather bad impression on the illustrious audience gathered for the occasion.

Born and de Broglie very quickly abandoned the pilot-wave approach and became enthusiastic supporters of the rapidly developing consensus in favor of the Copenhagen interpretation. Bohmian mechanics was rediscovered in 1952 by David Bohm (Bohm 1952), the first person genuinely to understand its significance and implications. Its principal proponent during the sixties, seventies and eighties was John Bell.

## 4. The Defining Equations of Bohmian Mechanics

In Bohmian mechanics the wave function, obeying Schrödinger's equation, does not provide a complete description or representation of a quantum system. Rather, it governs the motion of the fundamental variables, the positions of the particles: In the Bohmian mechanical version of nonrelativistic quantum theory, quantum mechanics is fundamentally about the behavior of particles; the particles are described by their positions, and Bohmian mechanics prescribes how these change with time. In this sense, for Bohmian mechanics the particles, described by their positions, are primary, or primitive, while the wave function is secondary, or derivative.

Warning: It is the positions of the particles in Bohmian mechanics that are its "hidden variables," an unfortunate bit of terminology. As Bell (1987, page 201) has written, referring to Bohmian mechanics and similar theories,

Absurdly, such theories are known as ‘hidden variable’ theories. Absurdly, for there it is not in the wavefunction that one finds an image of the visible world, and the results of experiments, but in the complementary ‘hidden’(!) variables. Of course the extra variables are not confined to the visible ‘macroscopic’ scale. For no sharp definition of such a scale could be made. The ‘microscopic’ aspect of the complementary variables is indeed hidden from us. But to admit things not visible to the gross creatures that we are is, in my opinion, to show a decent humility, and not just a lamentable addiction to metaphysics. In any case, the most hidden of all variables, in the pilot wave picture, is the wavefunction, which manifests itself to us only by its influence on the complementary variables.

Bohmian mechanics is the minimal completion of Schrödinger's
equation, for a nonrelativistic system of particles, to a theory
describing a genuine motion of particles. For Bohmian mechanics the
state of a system of *N* particles is described by its wave
function ψ =
ψ(*q*_{1},...,*q*_{
N}) = ψ(*q*), a complex (or
spinor) valued function on the space of possible configurations
*q* of the system, together with its actual configuration
*Q* defined by the actual positions
**Q**_{1},...,**Q**_{N}
of its particles. The theory is then defined by two evolution
equations: Schrödinger's equation

iℏ(∂ψ/∂t) =Hψ

for ψ(*t*), where *H* is the nonrelativistic
(Schrödinger) Hamiltonian, containing the masses of the particles
and a potential energy term, and a first-order evolution equation,

The Guiding Equation:

dQ_{k}/dt= (ℏ/m) Im [ψ*∂_{k}_{k}ψ/ ψ*ψ] (Q_{1},...,Q_{N})

for *Q(t)*, the simplest first-order evolution equation for the
positions of the particles that is compatible with the Galilean (and
time-reversal) covariance of the Schrödinger evolution (Dürr
et al. 1992, pp. 852-854). Here
ℏ
is
Planck's constant divided by 2π, *m _{k}* is the mass
of the

*k*-th particle, and ∂

_{k}is the gradient with respect to the coordinates of the

*k*-th particle. If ψ is spinor-valued, the products in numerator and denominator should be understood as scalar products. If external magnetic fields are present, the gradient should be understood as the covariant derivative, involving the vector potential. (Since the denominator on the right hand side of the guiding equation vanishes at the nodes of ψ, global existence and uniqueness for the Bohmian dynamics is a nontrivial matter. It is proven in Berndl, Dürr, et al. 1995 and in Teufel and Tumulka 2005.)

For an *N*-particle system these two equations (together with
the detailed specification of the Hamiltonian, including all
interactions contributing to the potential energy) completely define
the Bohmian mechanics. This deterministic theory of particles in motion
accounts for all the phenomena of nonrelativistic quantum mechanics,
from interference effects to spectral lines (Bohm 1952, pp. 175-178) to
spin (Bell 1964, p. 10), and it does so in an entirely ordinary manner,
as we shall explain in the following sections.

The form of the guiding equation given above is, for a scalar wave function, describing particles without spin, a little more complicated than necessary, since the complex conjugate of the wave function, appearing in the numerator and the denominator, cancels. If one looks for an evolution equation for the configuration compatible with the space-time symmetries of Schrödinger's equation, one almost immediately arrives at the guiding equation in this simpler form as the simplest possibility.

However, the form given above has two advantages: First, it makes
sense for particles with spin — and all the apparently
paradoxical quantum phenomena associated with spin are, in fact,
thereby accounted for by Bohmian mechanics without further ado.
Secondly, and this is crucial to the fact that Bohmian mechanics is
empirically equivalent to orthodox quantum theory, the right hand side
of the guiding equation is *J*/ρ, the ratio of the quantum
probability current to the quantum probability density. This shows
first of all that it should require no imagination whatsoever to guess
the guiding equation from Schrödinger's equation, provided one is
looking for one, since the classical formula for current is density
times velocity. Moreover, it follows from the quantum continuity
equation ∂ρ/∂*t* + div *J* = 0, an
immediate consequence of Schrödinger's equation, that if at some
time (say the initial time) the configuration *Q* of our system
is random, with distribution given by |ψ|^{2} =
ψ*ψ, this will be true at all times (so long as the system does
not interact with its environment).

This demonstrates that all claims to the effect that the predictions
of quantum theory are incompatible with the existence of hidden
variables, with an underlying deterministic model in which quantum
randomness arises from averaging over ignorance, are wrong. For Bohmian
mechanics provides us with just such a model:
For any quantum experiment we merely take as the
relevant Bohmian system the combined system that includes the system
upon which the experiment is performed as well as all the measuring
instruments and other devices used in performing the experiment
(together with all other systems with which these have significant
interaction over the course of the experiment). The "hidden variables"
model is then obtained by regarding the initial configuration of this
big system as random in the usual quantum mechanical way, with
distribution given by |ψ|^{2}. The initial configuration
is then transformed, via the guiding equation for the big system, into
the final configuration at the conclusion of the experiment. It then
follows that this final configuration of the big system, including in
particular the orientation of instrument pointers, will also be
distributed in the quantum mechanical way, so that this deterministic
Bohmian model yields the usual quantum predictions for the results of
the experiment.

As the preceding paragraph suggests, and as we discuss in more
detail in later sections, in Bohmian mechanics there is no need —
and, indeed, no room — for any "measurement postulates" or
*axioms* governing the behavior of other "observables": Any such
axioms would be at best redundant, and would quite possibly be
inconsistent.

## 5. The Quantum Potential

Bohmian mechanics has been presented here as a first-order theory, in which it is the velocity, the rate of change of position, that is fundamental: it is this quantity, given by the guiding equation, that is specified by the theory, directly and simply, with the second-order (Newtonian) concepts of acceleration and force, work and energy playing no fundamental role. Bohm, however, did not regard his theory in this way. He regarded it, fundamentally, as a second-order theory, describing particles moving under the influence of forces, among which, however, one must include a force stemming from a "quantum potential."

In his 1952 hidden-variables paper (Bohm 1952), Bohm arrived at his theory by writing the wave function in the polar form ψ =*R*exp(

*iS*/ℏ), where

*S*and

*R*are real, with

*R*nonnegative, and rewriting Schrödinger's equation in terms of these new variables to obtain a pair of coupled evolution equations: the continuity equation for ρ =

*R*and a modified Hamilton-Jacobi equation for

^{2}*S*, differing from the usual classical Hamilton-Jacobi equation only by the appearance of an extra term, the

*quantum potential*

U= −∑_{k}(ℏ^{2}/2m_{k}) (∂_{k}^{2}R/R),

alongside the classical potential energy term.

Bohm then used the modified Hamilton-Jacobi equation to define
particle trajectories just as is done for the classical Hamilton-Jacobi
equation, that is, by identifying ∂_{k}*S*
with
*m*_{k}*v*_{k},
i.e., by setting

dQ_{k}/dt= ∂_{k}S/m_{k},

which is equivalent to
the guiding equation
for
particles without spin. [Notice that in this form the guiding equation
is already suggested by the (pre-Schrödinger equation) de Broglie
relation ** p** =
ℏ

**, as well as by the eikonal equation of classical optics.] The resulting motion is precisely what would be obtained classically if the particles were acted upon by, in addition to the usual forces, the force generated by the quantum potential.**

*k*The quantum potential formulation of the de Broglie-Bohm theory is still fairly widely used. For example, the theory is presented in this way in the two existing monographs, by Bohm and Hiley and by Holland. And regardless of whether or not we regard the quantum potential as fundamental, it can in fact be quite useful. In order most simply to see that Newtonian mechanics should be expected to emerge from Bohmian mechanics in the classical limit, it is convenient to transform the theory into Bohm's Hamilton-Jacobi form. One then sees that the (size of the) quantum potential provides a measure of the deviation of Bohmian mechanics from its classical approximation. Moreover, the quantum potential can also be used to develop approximation schemes for solutions to Schrödinger's equation (Nerukh and Frederick 2000).

However, Bohm's rewriting of Schrödinger's equation in terms of variables that seem interpretable in classical terms does not come without a cost. The most obvious is increased complexity: Schrödinger's equation is rather simple, not to mention linear, whereas the modified Hamilton-Jacobi equation is somewhat complicated, and highly nonlinear — and still requires the continuity equation for its closure. The quantum potential itself is neither simple nor natural. Even to Bohm it has seemed "rather strange and arbitrary" (Bohm 1980, p. 80). And it is not very satisfying to think of the quantum revolution as amounting to the insight that nature is classical after all, except that there is in nature what appears to be a rather ad hoc additional force term, the one arising from the quantum potential. The artificiality suggested by the quantum potential is the price one pays if one insists on casting a highly nonclassical theory into a classical mold.

Moreover, the connection between classical mechanics and Bohmian
mechanics that is suggested by the quantum potential is rather
misleading. Bohmian mechanics is not simply classical mechanics with an
additional force term. In Bohmian mechanics the velocities are not
independent of positions, as they are classically, but are constrained
by the guiding equation. In classical Hamilton-Jacobi theory we also
have this equation for the velocity, but there the Hamilton-Jacobi
function *S* can be entirely eliminated and the description in
terms of *S* simplified and reduced to a finite-dimensional
description, with basic variables the positions and the (unconstrained)
momenta of all the particles, given by Hamilton's or Newton's
equations.

It can be argued that the most serious flaw in the quantum potential
formulation of Bohmian mechanics is that it gives a completely false
impression of the lengths to which we must go in order to convert
orthodox quantum theory into something more rational. The quantum
potential suggests, and indeed it has often been stated, that in order
to transform Schrödinger's equation into a theory that can, in
what are often called "realistic" terms, account for quantum phenomena,
many of which are dramatically nonlocal, we must add to the theory a
complicated quantum potential of a grossly nonlocal character. It
should be clear that such sentiments are inappropriate, since the
quantum potential need not be mentioned in the *formulation* of
Bohmian mechanics and in any case is merely a reflection of the wave
function, which Bohmian mechanics does not add to but shares with
orthodox quantum theory.

## 6. The Two-Slit Experiment

According to Richard Feynman, the two-slit experiment for electrons is
(Feynman et al. 1963, p. 37-2) "a phenomenon which is impossible,
*absolutely* impossible, to explain in any classical way, and
which has in it the heart of quantum mechanics. In reality it contains
the *only* mystery." This experiment (Feynman 1967, p. 130) "has
been designed to contain all of the mystery of quantum mechanics, to
put you up against the paradoxes and mysteries and peculiarities of
nature one hundred per cent." As to the question (Feynman 1967, p.
145), "How does it really work? What machinery is actually producing
this thing? Nobody knows any machinery. Nobody can give you a deeper
explanation of this phenomenon than I have given; that is, a
description of it."

But Bohmian mechanics is just such a deeper explanation. It resolves the dilemma of the appearance, in one and the same phenomenon, of both particle and wave properties in a rather straightforward manner: Bohmian mechanics is a theory of motion describing a particle (or particles) guided by a wave. Here we have a family of Bohmian trajectories for the two-slit experiment.

Figure 1: An ensemble of trajectories for the two-slit experiment, uniform in the slits.

(Adapted by Gernot Bauer from Philippidis et al. 1979.)

While each trajectory passes through but one of the slits, the wave passes through both; the interference profile that therefore develops in the wave generates a similar pattern in the trajectories guided by this wave.

Compare Feynman's presentation with Bell's (Bell 1987, p. 191):

Is it not clear from the smallness of the scintillation on the screen that we have to do with a particle? And is it not clear, from the diffraction and interference patterns, that the motion of the particle is directed by a wave? De Broglie showed in detail how the motion of a particle, passing through just one of two holes in screen, could be influenced by waves propagating through both holes. And so influenced that the particle does not go where the waves cancel out, but is attracted to where they cooperate. This idea seems to me so natural and simple, to resolve the wave-particle dilemma in such a clear and ordinary way, that it is a great mystery to me that it was so generally ignored.

The most puzzling aspect of the two-slit experiment is perhaps the following: If, by any means whatsoever, one is able to determine through which slit the particle passes, the interference pattern will be destroyed. This dramatic effect of observation is, in fact, a simple consequence of Bohmian mechanics. To see this one need only carefully consider what determining the slit through which the particle passes should mean. In particular, one must recognize that this must involve interaction with another system that must also be included in the Bohmian mechanical analysis. This destruction of interference is related, naturally enough, to the Bohmian mechanical analysis of quantum measurement (Bohm 1952), and it occurs via the mechanism that leads, in Bohmian mechanics, to the "collapse of the wave function."

## 7. The Measurement Problem

The most commonly cited of the conceptual difficulties that plague
quantum mechanics is the
measurement problem,
or, what amounts to more or less the same thing, the
paradox of Schrödinger's cat. Indeed, for many physicists the
measurement problem is not merely one of the conceptual difficulties of
quantum mechanics; it is *the* conceptual difficulty.

The problem is as follows. Suppose that the wave function of any individual system provides a complete description of that system. When we analyze the process of measurement in quantum mechanical terms, we find that the after-measurement wave function for system and apparatus arising from Schrödinger's equation for the composite system typically involves a superposition over terms corresponding to what we would like to regard as the various possible results of the measurement — e.g., different pointer orientations. It is difficult to discern in this description of the after-measurement situation the actual result of the measurement — e.g., some specific pointer orientation. But the whole point of quantum theory, and the reason we are to believe in it, is that it is supposed to provide a compelling, or at least an efficient, account of our observations, that is, of outcomes of measurements. In short, the measurement problem is this: Quantum theory implies that measurements typically fail to have outcomes of the sort the theory was created to explain.

By contrast, if, like Einstein, we regard the description provided by the wave function as incomplete, the measurement problem vanishes: With a theory or interpretation like Bohmian mechanics, in which the description of the after-measurement situation includes, in addition to the wave function, at least the values of the variables that register the result, there is no measurement problem. In Bohmian mechanics pointers always point.

The measurement problem is often expressed a little differently. It
is noted that textbook quantum theory provides two rules for the
evolution of the wave function of a quantum system: A deterministic
dynamics given by Schrödinger's equation for when the system is
not being "measured" or observed, and a random collapse of the wave
function to an *eigenstate* of the "measured observable" for
when it is. However, the objection continues, textbook quantum theory
does not provide a coherent account of how these two apparently
incompatible rules can be reconciled.

That this formulation of the measurement problem is more or less equivalent to the previous one should be reasonably clear: If a wave function provides a complete description of the after-measurement situation, the outcome of the measurement must correspond to a wave function describing the actual result, that is, a "collapsed" wave function. Hence the collapse rule. But it is difficult to take seriously the idea that those interactions between system and apparatus that we happen to call measurements should be governed by laws different from those governing all other interactions. Hence the apparently incompatibility of the two rules.

The second formulation of the measurement problem, though basically equivalent to the first one, suggests an important question: Can Bohmian mechanics itself provide a coherent account of how the two dynamical rules might be reconciled? How does Bohmian mechanics justify the use of the "collapsed" wave function in place of the original one? This question was answered in Bohm's first papers on Bohmian mechanics (Bohm 1952, Part I, Section 7, and Part II, Section 2). What would nowadays be called effects of decoherence, produced by interaction with the environment (air molecules, cosmic rays, internal microscopic degrees of freedom, etc.), make it extremely difficult for the component of the after-measurement wave function corresponding to the actual result of the measurement to develop significant overlap — in the configuration space of the very large system that includes all systems with which the original system and apparatus come into interaction — with the other components of the after-measurement wave function. But without such overlap the future evolution of the configuration of the system and apparatus is generated, to a high degree of accuracy, by that component all by itself. The replacement is thus justified as a practical matter. (See also Dürr et al. 1992, Section 5.)

It is widely believed by proponents of orthodox quantum theory that the measurement problem itself is somehow resolved by decoherence. It is not easy to understand this belief. In the first formulation of the measurement problem, nothing prevents us from including in the apparatus all sources of decoherence. But then there is no longer any room for decoherence to be in any way relevant to that argument. Be that as it may, one of the best descriptions of the mechanisms of decoherence, though not the word itself, was given by Bohm (Bohm 1952), who recognized its importance several decades before it became fashionable. (See also the encyclopedia entry on The Role of Decoherence in Quantum Mechanics.)

## 8. The Collapse of the Wave Function

In the previous section it was indicated that collapse of the wave
function can be regarded in Bohmian mechanics as a pragmatic affair.
However, there is a sense in which the collapse of the wave function in
Bohmian mechanics is more than a matter of convenience. If we focus on
what should be regarded as the wave function, not of the composite of
system and apparatus — which strictly speaking remains a
superposition if the composite is treated as closed during the
measurement process — but of the system itself, we find that for
Bohmian mechanics this does indeed collapse, precisely as described by
the quantum formalism. The key element here is the notion of the
*conditional wave function* of a subsystem of a larger system,
described briefly in this section and discussed in some detail,
together with the related notion of the effective wave function, in
Dürr et al. 1992, Section 5.

For the evolution of the wave function, Bohmian mechanics is
formulated in terms of Schrödinger's equation alone. Nonetheless
the textbook collapse rule is a consequence of the Bohmian dynamics. To
appreciate this one should first note that, since observation implies
interaction, a system under observation cannot be a closed system but
rather must be a subsystem of a larger system that is closed, which we
may take to be the entire universe, or any smaller more or less closed
system that contains the system to be observed, *the subsystem*.
The configuration *Q* of this larger system naturally splits
into *X*, the configuration of the subsystem, and *Y*,
the configuration of the *environment* of the subsystem.

Suppose the larger system has wave function Ψ =
Ψ(*q*) = Ψ(*x, y*). According to
Bohmian mechanics, the larger system is then completely described by
Ψ, evolving according to Schrödinger's equation, together with
*X* and *Y*. The question then arises — and it is a
critical question — as to what should be meant by the wave
function of the subsystem.

There is a rather obvious answer for this, a natural function of
*x* that suitably incorporates the objective structure at hand,
namely the *conditional wave function*

ψ(x) = Ψ(x,Y)

obtained by plugging the actual configuration of the environment into the wave function of the larger system. (This definition is appropriate only for scalar wave functions; for particles with spin the situation would be a little more complicated.) It then follows immediately that the configuration of the subsystem obeys the guiding equation with the conditional wave function on its right hand side.

Moreover, taking into account the way that the conditional wave
function depends upon time *t*

ψ_{t}(x) = Ψ_{t}(x,Y_{t})

via the time dependence of *Y* as well as that of Ψ, it is
not difficult to see (Dürr et al. 1992) that the conditional wave
function obeys Schrödinger's equation for the subsystem when that
system is suitably decoupled from its environment — this is meant
to imply, in particular, that Ψ has a special form, what might be
called an effective product form (similar to but more general than the
superposition produced in an "ideal quantum measurement"), in which
case the conditional wave function of the subsystem is also called its
*effective wave function* — and, using the
quantum equilibrium hypothesis,
that it randomly
collapses according to the usual quantum mechanical rules under
precisely those conditions on the interaction between the subsystem and
its environment that define an ideal quantum measurement.

It is perhaps worth noting that orthodox quantum theory lacks the resources, namely, the actual configuration of the environment, that make possible the definition of the conditional wave function. Indeed, from an orthodox point of view what should be meant by the wave function of a subsystem is entirely obscure.

## 9. Quantum Randomness

According to the quantum formalism, the probability density for
finding a system whose wave function is ψ in the configuration
*q* is |ψ(*q*)|^{2}. To the extent that the
results of measurement are registered configurationally, at least
potentially, it follows that the predictions of Bohmian mechanics for
the results of measurement must agree with those of orthodox quantum
theory (assuming the same Schrödinger equation for both) provided
that it is somehow true for Bohmian mechanics that configurations are
random, with distribution given by the *quantum equilibrium*
distribution |ψ(*q*)|^{2}. Now the status and
justification of this *quantum equilibrium hypothesis* is a
rather delicate matter, one that has been explored in considerable
detail (Dürr et al. 1992). Here are but a few relevant points.

It is nowadays a rather familiar fact that dynamical systems quite
generally give rise to behavior of a statistical character, with the
statistics given by the (or a) stationary probability distribution for
the dynamics. So it is with Bohmian mechanics, except that for the
Bohmian system stationarity is not quite the right concept, and it is
rather the notion of *equivariance* that is relevant. A
probability distribution ρ^{ψ} on configuration space,
depending upon the wave function ψ, is *equivariant* if

(ρ^{ψ})_{t}= ρ^{ψt}

where the dependence on *t* on the right arises from
Schrödinger's equation and on the left from the evolution on
probability distributions arising from the flow induced by
the guiding equation.
Thus equivariance expresses the
mutual compatibility, relative to ρ^{ψ}, of the
Schrödinger evolution of the wave function and the Bohmian motion
of the configuration. It is an immediate consequence of
the guiding equation
and the quantum continuity equation
that ρ^{ψ} = |ψ(*q*)|^{2} is
equivariant.

It is perhaps helpful, in trying to understand the status in Bohmian mechanics of the quantum equilibrium distribution, to think of

quantum equilibrium, ρ = |ψ|^{2}

as roughly analogous to (classical)

thermodynamic equilibrium, ρ = exp(-H/kT) /Z,

the probability distribution of the phase-space point of a system in
equilibrium at temperature *T*. (*Z* is a normalization
constant called the partition function and *k* is Boltzmann's
constant.) This analogy has several facets: In both cases the
probability distributions are naturally associated with their
respective dynamical systems. In particular, these distributions are
stationary or, what amounts to the same thing within the framework of
Bohmian mechanics, equivariant. In both cases it appears natural to try
to justify these equilibrium distributions by means of mixing-type,
convergence-to-equilibrium arguments (Bohm 1953, Valentini and Westman
2005). In both cases the ultimate justification for these probability
distributions must, arguably, be in terms of statistical patterns
exhibited by ensembles of actual subsystems within a *typical*
individual universe (Bell 1987, page 129, Dürr et al. 1992). (And
in both cases the status of, and justification for, equilibrium
distributions is still controversial. It is also perhaps worth noting
that the typicality-grounded account of quantum randomness in Bohmian
mechanics is extremely similar to Everett's account (Everett III 1957)
of quantum randomness for "many worlds," despite the huge metaphysical
differences between these two versions of quantum theory.) It can be
shown (Dürr et al. 1992) that probabilities for positions given by
the quantum equilibrium distribution emerge naturally from an analysis
of "equilibrium" for the deterministic dynamical system defined by
Bohmian mechanics, in much the same way that the Maxwellian velocity
distribution emerges from an analysis of classical thermodynamic
equilibrium. (For more on the thermodynamic side of the analogy see
Goldstein 2001.) Thus with Bohmian mechanics the statistical
description in quantum theory indeed takes, as Einstein anticipated,
"an approximately analogous position to the statistical mechanics
within the framework of classical mechanics."

## 10. Quantum Observables

It would appear that because orthodox quantum theory supplies us with probabilities not merely for positions but for a huge class of quantum observables, it is a much richer theory than Bohmian mechanics, which seems exclusively concerned with positions. Appearances are, however, misleading. In this regard, as with so much else in the foundations of quantum mechanics, the crucial remark has been made by Bell (Bell 1987, p. 166):

[I]n physics the only observations we must consider are position observations, if only the positions of instrument pointers. It is a great merit of the de Broglie-Bohm picture to force us to consider this fact. If you make axioms, rather than definitions and theorems, about the "measurement" of anything else, then you commit redundancy and risk inconsistency.

Consider first classical mechanics. The observables are functions on phase space, functions of the positions and momenta of the particles. The theory is defined by the axioms governing the behavior of the basic observables — Newton's equations for the positions or Hamilton's for positions and momenta. What would be the point of making additional axioms, for other observables? After all, the behavior of any observable is entirely determined by the behavior of the basic observables. For example, for classical mechanics, the principle of the conservation of energy is a theorem, not an axiom.

The situation might seem to be different in quantum mechanics, since in quantum mechanics there are no basic observables having the property that all other observables are functions of these. This is connected with the fact that in quantum mechanics, with its positivistic orientation, no observables are taken seriously as describing objective properties, as actually having values regardless of whether they are or have been measured. Rather, all talk of observables in quantum mechanics is supposed to be understood as talk about the measurement of the observables.

But if this is so, the situation with regard to other observables in quantum mechanics is not really that different from in classical mechanics. Whatever is supposed to be meant in quantum mechanics by the measurement of (the values of) observables — that, we are urged to believe, don't actually have values — it must at least refer to some experiment involving interaction between the "measured" system and a "measuring" apparatus leading to a recognizable result, as given potentially by, say, a pointer orientation. But then if the axioms that we do have suffice for the behavior of pointer orientations (at least when they are observed), rules about the measurement of other observables must be theorems, following from those axioms, not additional axioms.

It should be clear from the discussion
towards the end of Section 4
and at the
beginning of Section 9
that, assuming the quantum equilibrium hypothesis, any analysis of the
measurement of a quantum observable for orthodox quantum theory —
whatever that may be taken to mean and however the corresponding
experiment may be performed — provides ipso facto at least as
adequate an account for Bohmian mechanics. The only part of orthodox
quantum theory relevant to the analysis is the Schrödinger
evolution, and this it *shares* with Bohmian mechanics. The main
difference in the two accounts is that the orthodox one encounters
the measurement problem
before reaching a satisfactory
conclusion while the Bohmian account does not. This difference stems of
course from what Bohmian mechanics *adds* to orthodox quantum
theory: actual configurations.

In the rest of this section, I wish to touch upon the significance of quantum observables for Bohmian mechanics: on how they naturally emerge and what talk of them means. (It follows from what has been said in the three preceding paragraphs that what we conclude here about quantum observables for Bohmian mechanics holds for orthodox quantum theory as well.)

It happens that Bohmian mechanics leads to a natural association
between experiments and so-called *generalized observables*,
given by positive-operator-valued measures (Davies 1976), or POVM's,
*O*(*dz*), on the value spaces for the results of the
experiments (Berndl, Daumer, et al. 1995). This association is such
that the probability distribution of the result *Z* of an
experiment, when performed upon a system with wave function ψ, is
given by <ψ |
*O*(*dz*)ψ> (where < |
> is the usual
inner product
between quantum state vectors).

Moreover, this conclusion is basically an immediate consequence of
the very meaning of an experiment from a Bohmian perspective: a
coupling of system to apparatus leading to a result *Z* that is
a function of the final configuration of the total system, e.g., the
orientation of a pointer. Analyzed in Bohmian mechanical terms, the
experiment defines a map from the initial wave function of the system
to the distribution of the result. It follows directly from the
structure of Bohmian mechanics, and from the fact that the quantum
equilibrium distribution is quadratic in the wave function, that this
map is bilinear (or, more precisely, sesquilinear). Such a map is
equivalent to a POVM.

The simplest example of a POVM is a standard quantum observable,
corresponding to a self-adjoint operator *A* on the Hilbert
space of quantum states (i.e., wave functions). For Bohmian mechanics,
more or less every "measurement-like" experiment is associated with
this special kind of POVM, and the familiar quantum measurement axiom
that the distribution of the result of the "measurement of the
observable *A*" is given by the *spectral measure* for
*A* relative to the wave function (in the very simplest cases
just the absolute squares of the so-called *probability
amplitudes*) is thus obtained.

For a variety of reasons, it quickly became almost universal, after
quantum mechanics was discovered, to speak of an experiment associated
with an operator *A* in the manner just sketched as a
*measurement* of the *observable* *A*, as if the
operator somehow corresponded to a property of the system that is in
some sense measured by that experiment. There is no greater source of
confusion about the meaning and implications of quantum theory than
this
*naive realism about operators*
(Daumer et al., 1997).

## 11. Spin

Both the way non-configurational quantum observables are treated in Bohmian mechanics, and some of the difficulties caused by the naive realism about operators mentioned above, can be illustrated nicely with the case of spin.

Spin is the canonical quantum observable having no classical counterpart, reputed to be impossible to grasp in a nonquantum way. The source of the difficulty is not so much that spin is quantized in the sense that its allowable values form a discrete set (for a spin-1/2 particle, ±ℏ/2) — energy too may be quantized in this sense — nor even precisely that the components of spin in the different directions fail to commute and so cannot be simultaneously discussed, measured, imagined, or whatever it is that we are admonished not to do with noncommuting observables. Rather the difficulty is that there is no ordinary (nonquantum) quantity which, like the spin observable, is a 3-vector and which also is such that its components in all possible directions belong to the same discrete set. The problem, in other words, is that the usual vector relationships among the various components of the spin vector are incompatible with the quantization conditions on the values of these components.

For a particle of spin-1 the problem is even more severe. Since the components of spin in different directions aren't simultaneously measurable, the impossible vector relationships for the spin components of a quantum particle are not observable relationships. Simon Kochen and Ernst Specker (Kochen and Specker 1967) showed that for a spin-1 particle the squares of the spin components in the various directions satisfy, according to quantum theory, a collection of relationships, each individually observable, that taken together are impossible: the relationships are incompatible with the idea that measurements of these observables merely reveal their preexisting values rather than, as we are urged to believe in quantum theory, creating them. This Kochen-Specker Theorem continues to be regarded by many physicists and philosophers of physics as a definitive argument against the possibility of hidden variables.

We thus might naturally wonder how Bohmian mechanics manages to cope with spin. But this question has already been answered here. Bohmian mechanics makes sense for particles with spin, i.e., for particles whose wave functions are spinor-valued. When such particles are suitably directed toward Stern-Gerlach magnets, they emerge moving in more or less a discrete set of directions — 2 possible directions for a spin-1/2 particle, having 2 spin components, 3 for spin-1 with 3 spin components, and so on. This occurs because the Stern-Gerlach magnets are so designed and so oriented that a wave packet (a localized wave function with reasonably well defined velocity) directed towards the magnet will, by virtue of the Schrödinger evolution, separate into distinct packets — corresponding to the spin components of the wave function and moving in the discrete set of directions. The particle itself, depending upon its initial position, ends up in one of the packets moving in one of the directions.

The probability distribution for the result of such a
*Stern-Gerlach experiment* is conveniently expressed in terms of
the quantum mechanical spin operators — for a spin-1/2 particle
given by the Pauli spin matrices — in the manner alluded to
above.
From a Bohmian perspective there is no hint of
paradox in any of this unless we are seduced by naive realism about
operators into insisting, despite its evident impossibility, that the
spin operators correspond to genuine properties of the particles.

## 12. Contextuality

The
Kochen-Specker Theorem,
the
earlier theorem of Gleason (Gleason 1957 and Bell 1966), as well as a
variety of other no-hidden-variables results, including Bell's
inequality (Bell 1964), show that any hidden-variables formulation of
quantum mechanics must be *contextual*. It must violate the
noncontextuality assumption "that measurement of an observable must
yield the same value independently of what other measurements may be
made simultaneously" (Bell 1987, p. 9). To many physicists and
philosophers of science contextuality has seemed too great a price to
pay for the rather modest benefits — largely psychological, so
they would say — provided by hidden variables.

Even many Bohmians suggest that contextuality marks a significant departure from classical principles. For example, Bohm and Hiley (1993) write that "The context dependence of results of measurements is a further indication of how our interpretation does not imply a simple return to the basic principles of classical physics."

However, to understand contextuality from the perspective of Bohmian
mechanics is to appreciate that almost nothing needs to be explained.
Consider an operator *A* that commutes with operators *B*
and *C* (which however don't commute with each other). What is
often called the "result for *A*" in an experiment for
"measuring *A* together with *B*" usually disagrees with
the "result for *A*" in an experiment for "measuring *A*
together with *C*" because, even if everything else is the same,
these experiments are different and different experiments usually have
different results. The misleading reference to measurement, with the
associated naive realism about operators, makes contextuality seem more
than it is.

If we avoid naive realism about operators, contextuality amounts to
little more than the rather unremarkable observation that results of
experiments should depend upon how they are performed, even when the
experiments considered are associated with the same operator in the
manner alluded to
above.
David Albert (Albert 1992,
p. 153) has given a particularly simple and striking example of this
dependence for Stern-Gerlach experiments "measuring" the
*z*-component of spin. If one reverses the polarity in a magnet
for "measuring" the *z*-component of spin, keeping the same
geometry, one obtains another magnet for "measuring" the
*z*-component of spin. The use of one or the other of these two
magnets will often lead to opposite conclusions about the "value of the
*z*-component of spin" prior to the "measurement" (for the same
initial value of the position of the particle).

As Bell has insisted (Bell 1987, p. 166):

A final moral concerns terminology. Why did such serious people take so seriously axioms which now seem so arbitrary? I suspect that they were misled by the pernicious misuse of the word ‘measurement’ in contemporary theory. This word very strongly suggests the ascertaining of some preexisting property of some thing, any instrument involved playing a purely passive role. Quantum experiments are just not like that, as we learned especially from Bohr. The results have to be regarded as the joint product of ‘system’ and ‘apparatus,’ the complete experimental set-up. But the misuse of the word ‘measurement’ makes it easy to forget this and then to expect that the ‘results of measurements’ should obey some simple logic in which the apparatus is not mentioned. The resulting difficulties soon show that any such logic is not ordinary logic. It is my impression that the whole vast subject of ‘Quantum Logic’ has arisen in this way from the misuse of a word. I am convinced that the word ‘measurement’ has now been so abused that the field would be significantly advanced by banning its use altogether, in favour for example of the word ‘experiment.’

## 13. Nonlocality

Bohmian mechanics is manifestly nonlocal: The velocity, as expressed in the guiding equation, of any one of the particles of a many-particle system will typically depend upon the positions of the other, possibly distant, particles whenever the wave function of the system is entangled, i.e., not a product of single-particle wave functions. This is true, for example, for the EPR-Bohm wave function, describing a pair of spin-1/2 particles in the singlet state, analyzed by Bell and many others. Thus does Bohmian mechanics make explicit the most dramatic feature of quantum theory: quantum nonlocality.

It should be emphasized that the nonlocality of Bohmian mechanics derives solely from the nonlocality built into the structure of standard quantum theory, as provided by a wave function on configuration space, an abstraction which, roughly speaking, combines — or binds — distant particles into a single irreducible reality. As Bell (Bell 1987, p. 115) has stressed,

That the guiding wave, in the general case, propagates not in ordinary three-space but in a multidimensional-configuration space is the origin of the notorious ‘nonlocality’ of quantum mechanics. It is a merit of the de Broglie-Bohm version to bring this out so explicitly that it cannot be ignored.

Thus the nonlocal velocity relation in the guiding equation is but one aspect of the nonlocality of Bohmian mechanics. There is also the nonlocality, or nonseparability, implicit in the wave function itself and in its propagation, a nonlocality that does not in fact assume the structure — actual configurations — that Bohmian mechanics adds to orthodox quantum theory. And as Bell has shown, using the connection between the wave function and the predictions of quantum theory concerning experimental results, this nonlocality cannot easily be argued away (see Section 2).

The nonlocality of Bohmian mechanics can be appreciated perhaps most
efficiently, in all its aspects, by focusing on the
conditional wave function.
Suppose, for example, that
in an EPR-Bohm experiment particle 1 passes through its Stern-Gerlach
magnet before particle 2 arrives at its magnet. Then the orientation of
the Stern-Gerlach magnet for particle 1 will have a significant effect
upon the conditional wave function of particle 2: If the Stern-Gerlach
magnet for particle 1 is so oriented as to "measure the
*z*-component of spin," then after particle 1 has passed through
its magnet the conditional wave function of particle 2 will be an
eigenvector
(or eigenstate) of
the *z*-component of spin (in fact, belonging to the eigenvalue
that is the negative of the one "measured" for particle 1), and the
same thing is true for any other component of spin. You can dictate the
*kind* of spin eigenstate produced for particle 2 by
appropriately choosing the orientation of an arbitrarily distant
magnet. As to the future behavior of particle 2, in particular how it
is affected by its magnet, this of course depends very much on the
character of its conditional wave function and hence is very strongly
influenced by the choice of orientation of the distant magnet.

This nonlocal effect upon the conditional wave function of particle 2 follows from combining the standard analysis of the evolution of the wave function in the EPR-Bohm experiment with the definition of the conditional wave function. (For simplicity, we ignore permutation symmetry.) Before any magnets have been reached the EPR-Bohm wave function is a sum of two terms, corresponding to nonvanishing values for two of the four possible joint spin components for the two particles, each term a product of an eigenstate for a component of spin in a given direction for particle 1 with the opposite eigenstate (i.e., belonging to the eigenvalue that is the negative of the eigenvalue for particle 1) for the component of spin in the same direction for particle 2. Moreover, by virtue of its symmetry under rotations, it happens that the EPR-Bohm wave function has the property that any component of spin, i.e., any direction, can be used in this decomposition. (This property is very interesting.)

Decomposing the EPR-Bohm wave function using the component of spin in the direction associated with the magnet for particle 1, the evolution of the wave function as particle 1 passes its magnet is easy to grasp: The evolution of the sum is determined (using linearity) by that of its individual terms, and the evolution of each term by that of each of its factors. The evolution of the particle-1 factor leads to a displacement along the magnetic axis in the direction determined by the (sign of the) spin component (i.e., the eigenvalue), as described in the fourth paragraph of Section 11. Once this displacement has occurred (and is large enough) the conditional wave function for particle 2 will correspond to the term in the sum selected by the actual position of particle 1. In particular, it will be an eigenstate of the component of spin "measured by" the magnet for particle 1.

The nonlocality of Bohmian mechanics has a remarkable feature: it is screened by quantum equilibrium. It is a consequence of the quantum equilibrium hypothesis that the nonlocal effects in Bohmian mechanics don't yield observable consequences that are also controllable — we can't use them to send instantaneous messages. This follows from the fact that, given the quantum equilibrium hypothesis, the observable consequences of Bohmian mechanics are the same as those of orthodox quantum theory, for which instantaneous communication based on quantum nonlocality is impossible (see Eberhard 1978). The importance of quantum equilibrium for obscuring the nonlocality of Bohmian mechanics has been stressed by Valentini (1991).

## 14. Lorentz Invariance

Like nonrelativistic quantum theory, of which it is a version,
Bohmian mechanics is incompatible with special relativity, a central
principle of physics: it is not Lorentz invariant. Nor can Bohmian
mechanics easily be modified to become Lorentz invariant.
Configurations, defined by the *simultaneous* positions of all
particles, play too crucial a role in its formulation,
the guiding equation
defining an evolution on
*configuration* space. (Lorentz invariant extensions of Bohmian
mechanics for a single particle, described by the Dirac equation (Bohm
and Hiley 1993, Dürr et al. 1999) or the Klein-Gordon equation
(Berndl et al. 1996, Nikolic 2005), can easily be achieved, though for
a Klein-Gordon particle there are some interesting subtleties,
corresponding to what might seem to be a particle traveling backwards
in time.)

This difficulty with Lorentz invariance is intimately connected with the nonlocality in Bohmian mechanics. Since quantum theory itself, by virtue merely of the character of its predictions concerning EPR-Bohm correlations, is irreducibly nonlocal (see Section 2), one might expect considerable difficulty with the Lorentz invariance of orthodox quantum theory as well with Bohmian mechanics. For example, the collapse rule of textbook quantum theory blatantly violates Lorentz invariance. As a matter of fact, the intrinsic nonlocality of quantum theory presents formidable difficulties for the development of any (many-particle) Lorentz invariant formulation that avoids the vagueness of orthodox quantum theory (see Maudlin 1994).

A somewhat surprising, and I think correct, evaluation of the
importance of the problem of Lorentz invariance was made by Bell in an
interview with the philosopher Renée Weber, not long before he
died. Referring to the paradoxes of quantum mechanics, Bell observed
that "Those paradoxes are simply disposed of by the 1952 theory of
Bohm, leaving as *the* question, the question of Lorentz
invariance. So one of my missions in life is to get people to see that
if they want to talk about the problems of quantum mechanics —
the real problems of quantum mechanics — they must be talking
about Lorentz invariance."

The most common view on the matter of Lorentz invariance and quantum nonlocality is that a detailed description of microscopic quantum processes, such as would be provided by an extension of Bohmian mechanics to the relativistic domain, must violate Lorentz invariance. In this view Lorentz invariance is an emergent symmetry obeyed by our observations — a statistical consequence of quantum equilibrium that governs the results of quantum experiments. This is the opinion of Bohm and Hiley (1993), of Holland (1993), and of Valentini (2001).

However — unlike nonlocality — violation of Lorentz invariance is not inevitable. It should be possible, it seems, to construct a fully Lorentz invariant theory providing a detailed description of microscopic quantum processes. One way to do this is by means of additional Lorentz invariant dynamical structure, for example a suitable time-like 4-vector field, that permits the definition of a foliation of space-time into space-like hypersurfaces providing a Lorentz invariant notion of "evolving configuration" and along which nonlocal effects are transmitted. See Dürr et al. 1999 for a toy model. Another possibility that should not be dismissed is that a fully Lorentz invariant account of quantum nonlocality can be achieved without the invocation of additional structure, exploiting only what is already at hand, for example, light-cone structure. For a step in this direction, a model in which the reconciliation of relativity and nonlocality is achieved through the interplay of opposite arrows of time, see Goldstein and Tumulka 2003.

Be that as it may, Lorentz invariant nonlocality would remain
somewhat enigmatic. The issues are extremely subtle. For example, Bell
(1987, page 155) rightly would find "disturbing ... the impossibility
of ‘messages’ faster than light, which follows from
ordinary relativistic quantum mechanics in so far as it is unambiguous
and adequate for procedures *we* [emphasis added] can actually
perform. The exact elucidation of concepts like ‘message’
and ‘we’, would be a formidable challenge." While quantum
equilibrium and the absolute uncertainty that it entails (Dürr et
al. 1992) may be of some help here, the situation remains puzzling.

## 15. Objections

Anyone who has engaged in arguments with colleagues about the foundations of quantum mechanics, whatever his position, will likely agree with the following observation of Tolstoy:

I know that most men, including those at ease with problems of the highest complexity, can seldom accept even the simplest and most obvious truth if it be such as would oblige them to admit the falsity of conclusions which they have delighted in explaining to colleagues, which they have proudly taught to others, and which they have woven, thread by thread, into the fabric of their lives.

A great many objections have been and continue to be raised against
Bohmian mechanics. Here are some of them: Bohmian mechanics makes
predictions about results of experiments different from those of
orthodox quantum theory so it is wrong. Bohmian mechanics makes the
same predictions about results of experiments as orthodox quantum
theory so it is untestable and therefore meaningless. Bohmian mechanics
is mathematically equivalent to orthodox quantum theory so it is not
really an alternative at all. Bohmian mechanics is more complicated
than orthodox quantum theory, since it involves an extra equation.
(This objection is based on the surprisingly common misconception that
orthodox quantum theory is defined solely by Schrödinger's
equation, and does not actually need as part of its formulation any of
the measurement postulates found in textbook quantum theory. It is only
within a
many-worlds
framework that
this view could begin to make sense, but I strongly doubt that it makes
sense even there.) Bohmian mechanics requires the postulation of a
mysterious and undetectable quantum potential. Bohmian mechanics
requires the addition to quantum theory of a mysterious pilot wave.
Bohmian mechanics, as von Neumann has shown, can't possibly work.
Bohmian mechanics, as Kochen and Specker have shown, can't possibly
work. Bohmian mechanics, as Bell has shown, can't possibly work.
Bohmian mechanics is a childish regression to discredited classical
modes of thought. Bohmian trajectories are crazy, since they may be
curved even when no classical forces are present. Bohmian trajectories
are crazy, since a Bohmian particle may be at rest in stationary
quantum states. Bohmian trajectories are crazy, since a Bohmian
particle may be at rest in stationary quantum states, even when these
are large-energy eigenstates. Bohmian trajectories are surrealistic.
Bohmian mechanics, since it is deterministic, is incompatible with
quantum randomness. Bohmian mechanics is nonlocal. Bohmian mechanics is
unintuitive. Bohmian mechanics is the many-worlds interpretation in
disguise. (For a bit of discussion of some of these objections, see the
exchange of letters on Quantum Theory Without Observers, in the
February 1999 issue of *Physics Today*, particularly the last
four of the eight letters. A link is provided in the
Other Internet Resources
section below.)

Most of these objections have little or no merit. Some arise from naive realism about operators, some from the idea that, to the extent that the concepts of classical physics apply at all, the laws of classical physics are more or less a priori, some from an inability to grasp the point of Bohmian mechanics, and some from sheer ignorance. One common objection brings to mind a confession of Hilary Putnam (2005), who wrote that

In Putnam ([1965]), I rejected Bohm's interpretation for several reasons which no longer seem good to me. Even today, if you look at the Wikipedia encyclopaedia on the Web, you will find it said that Bohm's theory is mathematically inelegant. Happily, I did not give that reason in Putnam ([1965]), but in any case it is not true. The formula for the velocity field is extremely simple: you have the probability current in the theory anyway, and you take the velocity vector to be proportional to the current. There is nothing particularly inelegant about that; if anything, it is remarkably elegant!

Some recent objections are baffling. For example, referring to the measurement problem, Sir Anthony Leggett, 2003 Nobel Laureate in Physics, says that Bohmian mechanics provides (Leggett 2005) "little more than verbal window dressing of the basic paradox." No explanation is given, but elsewhere Leggett (2003) writes, in response to the Bohmian resolution of the puzzles of the two-slit experiment, that "No experimental consequences are drawn from [the Bohmian description] other than the standard predictions of the QM formalism, so whether one regards it as a substantive resolution of the apparent paradox or as little more than a reformulation of it is no doubt a matter of personal taste (the present author inclines towards the latter point of view)." In a similar vein, Sir Roger Penrose (2005, page 811) has written that "it seems to me that some measure of scale is indeed needed, for defining when classical-like behaviour begins to take over from small-scale quantum activity. In common with the other quantum ontologies in which no measurable deviations from standard quantum mechanics is expected, the point of view (e) [Bohmian mechanics] does not possess such a scale measure, so I do not see that it can adequately address the paradox of Schrödinger's cat."

The Bohmian account of the two-slit experiment, in Section 6, and its resolution of the measurement problem (or the paradox of Schrödinger's cat), in Section 7, are simple and straightforward. With regard to the latter, in Bohmian mechanics particles always have definite positions, and hence pointers, which are made of particles, always point. Thus the objections of Leggett and Penrose are hard to fathom. Leggett apparently bases his objection on the empirical equivalence of Bohmian mechanics and orthodox quantum theory. In so doing he seems to have forgotten the point of the measurement problem, i.e., that for orthodox quantum theory to yield any predictions at all, it must invoke a special dynamics just for measurement processes (collapse of the wave packet), one that conflicts with the fundamental Schrödinger dynamics. This is an expedient that Bohmian mechanics entirely avoids.

As to Penrose, contrary to what he writes, his real concern seems to be with the emergence of classical behavior, and not with the measurement problem per se. With regard to this, we note that the Bohmian evolution of particles, which is always governed by the wave function and is always fundamentally quantum, turns out to be approximately classical when the relevant de Broglie wave length, determined in part by the wave function, is much smaller than the scale on which the potential energy term in Schrödinger's equation varies (see Allori et al., 2002). Under normal circumstances this condition will be satisfied for the center of mass motion of a macroscopic object.

It is perhaps worth mentioning that despite the empirical equivalence between Bohmian mechanics and orthodox quantum theory, there are a variety of experiments and experimental issues that don't fit comfortably within the standard quantum formalism but are easily handled by Bohmian mechanics. Among these are dwell and tunneling times (Leavens 1996), escape times and escape positions (Daumer et al. 1997a), scattering theory (Dürr et al., 2000), and quantum chaos (Cushing 1994, Dürr et al., 1992a).

There is one striking feature of Bohmian mechanics that is often
presented as an objection but is better regarded as an important clue
about the meaning of quantum mechanics: in Bohmian mechanics the wave
function acts upon the positions of the particles but, evolving as it
does autonomously via Schrödinger's equation, it is not acted upon
by the particles. This point is discussed in Dürr *et al.*
1997 and in Goldstein and Teufel 2001, where it is suggested that, from
a deeper perspective than afforded by standard Bohmian mechanics or
quantum theory, the wave function should be regarded as nomological, as
an object for conveniently expressing the law of motion somewhat
analogous to the Hamiltonian in classical mechanics, and that a
time-dependent Schrödinger-type equation, from this deeper
(cosmological) perspective, is merely phenomenological.

Bohmian mechanics does not account for phenomena such as particle creation and annihilation characteristic of quantum field theory. This is not an objection to Bohmian mechanics but merely a recognition that quantum field theory explains a great deal more than does nonrelativistic quantum mechanics, whether in orthodox or Bohmian form. It does, however, underline the need to find an adequate, if not compelling, Bohmian version of quantum field theory, and of gauge theories in particular. Some rather tentative steps in this direction can be found in Bohm and Hiley 1993, Holland 1993, Bell 1987 (p. 173), and in some of the articles in Cushing et al. 1996. A crucial issue is whether a quantum field theory is fundamentally about fields or particles — or something else entirely. While the most common choice is fields, Bell's is particles. His proposal is in fact the basis of a canonical extension of Bohmian mechanics to general quantum field theories, and these "Bell-type quantum field theories" (Dürr et al., 2004 and 2005) describe a stochastic evolution of particles that involves particle creation and annihilation. (For a general discussion of this issue, and of the point and value of Bohmian mechanics, see the exchange of letters between Goldstein and Weinberg by following the link provided in the Other Internet Resources section below.)

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## Other Internet Resources

- Collaboration Bohmian Mechanics
- Bohmian Mechanics at the University of Innsbruck
- Pablo Yepes' Double Slit Experiment Simulator
- The "Mt. Rushmore" of foundations of quantum theory
- Chris Dewdney's de Broglie — Bohm website
- Eric Dennis' discussion e-group on Bell's inequality and Bohmian mechanics
- Exchange of letters on Quantum Theory Without Observers,
(reprinted from
*Physics Today*, February 1999)

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Einstein, Albert: Einstein-Bohr debates | physics: holism and nonseparability | quantum mechanics | quantum mechanics: Copenhagen interpretation of | quantum mechanics: Kochen-Specker theorem | quantum mechanics: many-worlds interpretation of | quantum mechanics: modal interpretations of | quantum mechanics: the role of decoherence in | quantum theory: measurement in | quantum theory: quantum entanglement and information | quantum theory: quantum gravity | quantum theory: quantum logic and probability theory | quantum theory: the Einstein-Podolsky-Rosen argument in | Uncertainty Principle

### Acknowledgments

I am grateful to the subject editor, Guido Bacciagaluppi, for a very careful reading and many valuable suggestions.