# Wigner–Weyl transform

In quantum mechanics, the Wigner–Weyl transform or Weyl–Wigner transform (after Hermann Weyl and Eugene Wigner) is the invertible mapping between functions in the quantum phase space formulation and Hilbert space operators in the Schrödinger picture.

Often the mapping from functions on phase space to operators is called the Weyl transform or Weyl quantization, whereas the inverse mapping, from operators to functions on phase space, is called the Wigner transform. This mapping was originally devised by Hermann Weyl in 1927 in an attempt to map symmetrized classical phase space functions to operators, a procedure known as Weyl quantization.[1] It is now understood that Weyl quantization does not satisfy all the properties one would require for consistent quantization and therefore sometimes yields unphysical answers. On the other hand, some of the nice properties described below suggest that if one seeks a single consistent procedure mapping functions on the classical phase space to operators, the Weyl quantization is the best option: a sort of normal coordinates of such maps. (Groenewold's theorem asserts that no such map can have all the ideal properties one would desire.)

Regardless, the Weyl–Wigner transform is a well-defined integral transform between the phase-space and operator representations, and yields insight into the workings of quantum mechanics. Most importantly, the Wigner quasi-probability distribution is the Wigner transform of the quantum density matrix, and, conversely, the density matrix is the Weyl transform of the Wigner function.

In contrast to Weyl's original intentions in seeking a consistent quantization scheme, this map merely amounts to a change of representation within quantum mechanics; it need not connect "classical" with "quantum" quantities. For example, the phase-space function may depend explicitly on Planck's constant ħ, as it does in some familiar cases involving angular momentum. This invertible representation change then allows one to express quantum mechanics in phase space, as was appreciated in the 1940s by Hilbrand J. Groenewold[2] and José Enrique Moyal.[3][4]

## Definition of the Weyl quantization of a general observable

The following explains the Weyl transformation on the simplest, two-dimensional Euclidean phase space. Let the coordinates on phase space be (q,p), and let f be a function defined everywhere on phase space. In what follows, we fix operators P and Q satisfying the canonical commutation relations, such as the usual position and momentum operators in the Schrödinger representation. We assume that the exponentiated operators ${\displaystyle e^{iaQ}}$ and ${\displaystyle e^{ibP}}$ constitute an irreducible representation of the Weyl relations, so that the Stone–von Neumann theorem (guaranteeing uniqueness of the canonical commutation relations) holds.

### The basic formula

The Weyl transform (or Weyl quantization) of the function f is given by the following operator in Hilbert space,

${\displaystyle \Phi [f]={\frac {1}{(2\pi )^{2}}}\iint \!\!\!\iint f(q,p)\left(e^{i(a(Q-q)+b(P-p))}\right){\text{d}}q\,{\text{d}}p\,{\text{d}}a\,{\text{d}}b.}$

Throughout, ${\displaystyle \hbar }$ is the reduced Planck constant.

It is instructive to perform the p and q integrals in the above formula first, which has the effect of computing the ordinary Fourier transform ${\displaystyle {\tilde {f}}}$ of the function ${\displaystyle f}$, while leaving the operator ${\displaystyle e^{i(aQ+bP)}}$. In that case, the Weyl transform can be written as[5]

${\displaystyle \Phi [f]={\frac {1}{(2\pi )^{2}}}\iint {\tilde {f}}(a,b)e^{iaQ+ibP}\,da\,db}$.

We may therefore think of the Weyl map as follows: We take the ordinary Fourier transform of the function ${\displaystyle f(p,q)}$, but then when applying the Fourier inversion formula, we substitute the quantum operators ${\displaystyle P}$ and ${\displaystyle Q}$ for the original classical variables ${\displaystyle p}$ and ${\displaystyle q}$, thus obtaining a "quantum version of ${\displaystyle f}$."

A less symmetric form, but handy for applications, is the following,

${\displaystyle \Phi [f]={\frac {2}{(2\pi \hbar )^{3/2}}}\iint \!\!\!\iint \!\!dqdpd{\tilde {x}}d{\tilde {p}}~e^{{\frac {i}{\hbar }}({\tilde {x}}{\tilde {p}}-2({\tilde {p}}-p)({\tilde {x}}-q))}~f(q,p)~|{\tilde {x}}\rangle \langle {\tilde {p}}|.}$

### In the position representation

The Weyl map may then also be expressed in terms of the integral kernel matrix elements of this operator,[6]

${\displaystyle \langle x|\Phi [f]|y\rangle =\int _{-\infty }^{\infty }{{\text{d}}p \over h}~e^{ip(x-y)/\hbar }~f\left({x+y \over 2},p\right).}$

### The inverse map

The inverse of the above Weyl map is the Wigner map, which takes the operator Φ back to the original phase-space kernel function f,

${\displaystyle f(q,p)=2\int _{-\infty }^{\infty }{\text{d}}y~e^{-2ipy/\hbar }~\langle q+y|\Phi [f]|q-y\rangle .}$

For example, the Wigner map of the oscillator thermal distribution operator ${\displaystyle \exp(-\beta (P^{2}+Q^{2})/2)}$ is[7]

${\displaystyle \exp _{\star }\left(-\beta (p^{2}+q^{2})/2\right)=\left(\cosh({\frac {\beta \hbar }{2}})\right)^{-1}\exp \left({\frac {-2}{\hbar }}\tanh({\frac {\beta \hbar }{2}})(p^{2}+q^{2})/2\right).}$

If one replaces ${\displaystyle \Phi [f]}$ in the above expression with an arbitrary operator, the resulting function f may depend on Planck's constant ħ, and may well describe quantum-mechanical processes, provided it is properly composed through the star product, below.[8] In turn, the Weyl map of the Wigner map is summarized by Groenewold's formula,[7]

${\displaystyle \Phi [f]=h\iint \,da\,db~e^{iaQ+ibP}\operatorname {Tr} (e^{-iaQ-ibP}\Phi ).}$

### The Weyl quantization of polynomial observables

While the above formulas give a nice understanding of the Weyl quantization of a very general observable on phase space, they are not very convenient for computing on simple observables, such as those that are polynomials in ${\displaystyle q}$ and ${\displaystyle p}$. In later sections, we will see that on such polynomials, the Weyl quantization represents the totally symmetric ordering of the noncommuting operators ${\displaystyle Q}$ and ${\displaystyle P}$. For example, the Wigner map of the quantum angular-momentum-squared operator L2 is not just the classical angular momentum squared, but it further contains an offset term −3ħ2/2, which accounts for the nonvanishing angular momentum of the ground-state Bohr orbit.

## Properties

### Weyl quantization of polynomials

The action of the Weyl quantization on polynomial functions of ${\displaystyle q}$ and ${\displaystyle p}$ is completely determined by the following symmetric formula:[9]

${\displaystyle (aq+bp)^{n}\longmapsto (aQ+bP)^{n}}$

for all complex numbers ${\displaystyle a}$ and ${\displaystyle b}$. From this formula, it is not hard to show that the Weyl quantization on a function of the form ${\displaystyle q^{k}p^{l}}$ gives the average of all possible orderings of ${\displaystyle k}$ factors of ${\displaystyle Q}$ and ${\displaystyle l}$ factors of ${\displaystyle P}$. For example, we have

${\displaystyle 6p^{2}q^{2}~~\longmapsto ~~P^{2}Q^{2}+Q^{2}P^{2}+PQPQ+PQ^{2}P+QPQP+QP^{2}Q.}$

While this result is conceptually natural, it is not convenient for computations when ${\displaystyle k}$ and ${\displaystyle l}$ are large. In such cases, we can use instead McCoy's formula[10]

${\displaystyle p^{m}q^{n}~~\longmapsto ~~{1 \over 2^{n}}\sum _{r=0}^{n}{n \choose r}Q^{r}P^{m}Q^{n-r}={1 \over 2^{m}}\sum _{s=0}^{m}{m \choose s}P^{s}Q^{n}P^{m-s}.}$

This expression gives an apparently different answer for the case of ${\displaystyle p^{2}q^{2}}$ from the totally symmetric expression above. There is no contradiction, however, since the canonical commutation relations allow for more than one expression for the same operator. (The reader may find it instructive to use the commutation relations to rewrite the totally symmetric formula for the case of ${\displaystyle p^{2}q^{2}}$ in terms of the operators ${\displaystyle P^{2}Q^{2}}$, ${\displaystyle QP^{2}Q}$, and ${\displaystyle Q^{2}P^{2}}$ and verify the first expression in McCoy's formula with ${\displaystyle m=n=2}$.)

It is widely thought that the Weyl quantization, among all quantization schemes, comes as close as possible to mapping the Poisson bracket on the classical side to the commutator on the quantum side. (An exact correspondence is impossible, in light of Groenewold's theorem.) For example, Moyal showed the

Theorem: If ${\displaystyle f(q,p)}$ is a polynomial of degree at most 2 and ${\displaystyle g(q,p)}$ is an arbitrary polynomial, then we have ${\displaystyle \Phi (\{f,g\})={\frac {1}{i\hbar }}[\Phi (f),\Phi (g)]}$.

## Deformation quantization

Intuitively, a deformation of a mathematical object is a family of the same kind of objects that depend on some parameter(s). Here, it provides rules for how to deform the "classical" commutative algebra of observables to a quantum non-commutative algebra of observables.

The basic setup in deformation theory is to start with an algebraic structure (say a Lie algebra) and ask: Does there exist a one or more parameter(s) family of similar structures, such that for an initial value of the parameter(s) one has the same structure (Lie algebra) one started with? (The oldest illustration of this may be the realization of Eratosthenes in the ancient world that a flat earth was deformable to a spherical earth, with deformation parameter 1/R.) E.g., one may define a noncommutative torus as a deformation quantization through a -product to implicitly address all convergence subtleties (usually not addressed in formal deformation quantization). Insofar as the algebra of functions on a space determines the geometry of that space, the study of the star product leads to the study of a non-commutative geometry deformation of that space.

In the context of the above flat phase-space example, the star product (Moyal product, actually introduced by Groenewold in 1946), ħ, of a pair of functions in f1, f2C(ℜ2), is specified by

${\displaystyle \Phi [f_{1}\star f_{2}]=\Phi [f_{1}]\Phi [f_{2}].\,}$

The star product is not commutative in general, but goes over to the ordinary commutative product of functions in the limit of ħ → 0. As such, it is said to define a deformation of the commutative algebra of C(ℜ2).

For the Weyl-map example above, the -product may be written in terms of the Poisson bracket as

${\displaystyle f_{1}\star f_{2}=\sum _{n=0}^{\infty }{\frac {1}{n!}}\left({\frac {i\hbar }{2}}\right)^{n}\Pi ^{n}(f_{1},f_{2}).}$

Here, Π is the Poisson bivector, an operator defined such that its powers are

${\displaystyle \Pi ^{0}(f_{1},f_{2})=f_{1}f_{2}}$

and

${\displaystyle \Pi ^{1}(f_{1},f_{2})=\{f_{1},f_{2}\}={\frac {\partial f_{1}}{\partial q}}{\frac {\partial f_{2}}{\partial p}}-{\frac {\partial f_{1}}{\partial p}}{\frac {\partial f_{2}}{\partial q}}~,}$

where {f1, f2} is the Poisson bracket. More generally,

${\displaystyle \Pi ^{n}(f_{1},f_{2})=\sum _{k=0}^{n}(-1)^{k}{n \choose k}\left({\frac {\partial ^{k}}{\partial p^{k}}}{\frac {\partial ^{n-k}}{\partial q^{n-k}}}f_{1}\right)\times \left({\frac {\partial ^{n-k}}{\partial p^{n-k}}}{\frac {\partial ^{k}}{\partial q^{k}}}f_{2}\right)}$

where ${\displaystyle {n \choose k}}$ is the binomial coefficient.

Thus, e.g.,[7] Gaussians compose hyperbolically,

${\displaystyle \exp \left(-{a}(q^{2}+p^{2})\right)~\star ~\exp \left(-{b}(q^{2}+p^{2})\right)={1 \over 1+\hbar ^{2}ab}\exp \left(-{a+b \over 1+\hbar ^{2}ab}(q^{2}+p^{2})\right),}$

or

${\displaystyle \delta (q)~\star ~\delta (p)={2 \over h}\exp \left(2i{qp \over \hbar }\right),}$

etc. These formulas are predicated on coordinates in which the Poisson bivector is constant (plain flat Poisson brackets). For the general formula on arbitrary Poisson manifolds, cf. the Kontsevich quantization formula.

Antisymmetrization of this -product yields the Moyal bracket, the proper quantum deformation of the Poisson bracket, and the phase-space isomorph (Wigner transform) of the quantum commutator in the more usual Hilbert-space formulation of quantum mechanics. As such, it provides the cornerstone of the dynamical equations of observables in this phase-space formulation.

There results a complete phase space formulation of quantum mechanics, completely equivalent to the Hilbert-space operator representation, with star-multiplications paralleling operator multiplications isomorphically.[7]

Expectation values in phase-space quantization are obtained isomorphically to tracing operator observables Φ with the density matrix in Hilbert space: they are obtained by phase-space integrals of observables such as the above f with the Wigner quasi-probability distribution effectively serving as a measure.

Thus, by expressing quantum mechanics in phase space (the same ambit as for classical mechanics), the above Weyl map facilitates recognition of quantum mechanics as a deformation (generalization, cf. correspondence principle) of classical mechanics, with deformation parameter ħ/S. (Other familiar deformations in physics involve the deformation of classical Newtonian into relativistic mechanics, with deformation parameter v/c; or the deformation of Newtonian gravity into General Relativity, with deformation parameter Schwarzschild-radius/characteristic-dimension. Conversely, group contraction leads to the vanishing-parameter undeformed theories—classical limits.)

Classical expressions, observables, and operations (such as Poisson brackets) are modified by ħ-dependent quantum corrections, as the conventional commutative multiplication applying in classical mechanics is generalized to the noncommutative star-multiplication characterizing quantum mechanics and underlying its uncertainty principle.

Despite its name, Deformation Quantization does not constitute a successful quantization scheme, namely a method to produce a quantum theory out of a classical one. It amounts to a mere representation change from Hilbert space to phase space.

## Generalizations

In more generality, Weyl quantization is studied in cases where the phase space is a symplectic manifold, or possibly a Poisson manifold. Related structures include the Poisson–Lie groups and Kac–Moody algebras.

## References

1. ^ Weyl, H. (1927). "Quantenmechanik und Gruppentheorie". Zeitschrift für Physik. 46 (1–2): 1–46. Bibcode:1927ZPhy...46....1W. doi:10.1007/BF02055756. S2CID 121036548.
2. ^ Groenewold, H. J. (1946). "On the Principles of elementary quantum mechanics". Physica. 12 (7): 405–446. Bibcode:1946Phy....12..405G. doi:10.1016/S0031-8914(46)80059-4.
3. ^ Moyal, J. E.; Bartlett, M. S. (1949). "Quantum mechanics as a statistical theory". Mathematical Proceedings of the Cambridge Philosophical Society. 45 (1): 99–124. Bibcode:1949PCPS...45...99M. doi:10.1017/S0305004100000487.
4. ^ Curtright, T. L.; Zachos, C. K. (2012). "Quantum Mechanics in Phase Space". Asia Pacific Physics Newsletter. 1: 37–46. arXiv:1104.5269. doi:10.1142/S2251158X12000069. S2CID 119230734.
5. ^ Hall 2013 Section 13.3
6. ^ Hall 2013 Definition 13.7
7. ^ a b c d Curtright, T. L.; Fairlie, D. B.; Zachos, C. K. (2014). A Concise Treatise on Quantum Mechanics in Phase Space. World Scientific. ISBN 9789814520430.
8. ^ Kubo, R. (1964). "Wigner Representation of Quantum Operators and Its Applications to Electrons in a Magnetic Field". Journal of the Physical Society of Japan. 19 (11): 2127–2139. Bibcode:1964JPSJ...19.2127K. doi:10.1143/JPSJ.19.2127.
9. ^ Hall 2013 Proposition 13.3
10. ^ McCoy, Neal (1932). "On the Function in Quantum Mechanics which Corresponds to a Given Function in Classical Mechanics", Proc Nat Acad Sci USA 19 674, online .
• Hall, Brian C. (2013), Quantum Theory for Mathematicians, Graduate Texts in Mathematics, 267, Springer, ISBN 978-1461471158