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In mathematics and classical mechanics, the **Poisson bracket** is an important binary operation in Hamiltonian mechanics, playing a central role in Hamilton's equations of motion, which govern the time-evolution of a Hamiltonian dynamical system. The Poisson bracket also distinguishes a certain class of coordinate-transformations, called *canonical transformations*, which maps canonical coordinate systems into canonical coordinate systems. (A "canonical coordinate system" consists of canonical position and momentum variables that satisfy canonical Poisson-bracket relations.) The set of possible canonical transformations is always very rich. For instance, often it is possible to choose the Hamiltonian itself *H* = *H*(*q*, *p*; *t*) as one of the new canonical momentum coordinates.

In a more general sense: the Poisson bracket is used to define a Poisson algebra, of which the algebra of functions on a Poisson manifold is a special case. These are all named in honour of Siméon Denis Poisson.

In canonical coordinates (also known as Darboux coordinates) on the phase space, given two functions and , the Poisson bracket takes the form

Hamilton's equations of motion have an equivalent expression in terms of the Poisson bracket. This may be most directly demonstrated in an explicit coordinate frame. Suppose that *f* (*p*, *q*, *t*) is a function on the manifold. Then from the multivariable chain rule, one has

Further, one may take *p* = *p*(*t*) and *q* = *q*(*t*) to be solutions to Hamilton's equations; that is,

Then, one has

Thus, the time evolution of a function f on a symplectic manifold can be given as a one-parameter family of symplectomorphisms (i.e. canonical transformations, area-preserving diffeomorphisms), with the time *t* being the parameter: Hamiltonian motion is a canonical transformation generated by the Hamiltonian. That is, Poisson brackets are preserved in it, so that *any time t* in the solution to Hamilton's equations, *q*(*t*)=exp(−*t*{*H*,•}) *q*(0), *p*(*t*)=exp(−*t*{*H*,•}) *p*(0), can serve as the bracket coordinates. *Poisson brackets are canonical invariants*.

Dropping the coordinates, one has

The operator in the convective part of the derivative, i*L̂* = −{*H*, •} , is sometimes referred to as the Liouvillian (see Liouville's theorem (Hamiltonian)).

An integrable dynamical system will have constants of motion in addition to the energy. Such constants of motion will commute with the Hamiltonian under the Poisson bracket. Suppose some function *f(p,q)* is a constant of motion. This implies that if *p(t)*, *q(t)* is a trajectory or solution to the Hamilton's equations of motion, then one has that

along that trajectory. Then one has

where, as above, the intermediate step follows by applying the equations of motion. This equation is known as the Liouville equation. The content of Liouville's theorem is that the time evolution of a measure (or "distribution function" on the phase space) is given by the above.

If the Poisson bracket of *f* and *g* vanishes (*{f,g}* = 0), then *f* and *g* are said to be **in involution**. In order for a Hamiltonian system to be completely integrable, all of the constants of motion must be in mutual involution.

Let *M* be symplectic manifold, that is, a manifold equipped with a symplectic form: a 2-form ω which is both **closed** (i.e. its exterior derivative *d*ω = 0) and **non-degenerate**. For example, in the treatment above, take *M* to be and take

If is the interior product or contraction operation defined by , then non-degeneracy is equivalent to saying that for every one-form α there is a unique vector field Ω_{α} such that . Then if *H* is a smooth function on *M*, the Hamiltonian vector field *X _{H}* can be defined to be . It is easy to see that

The **Poisson bracket** on (*M*, ω) is a bilinear operation on differentiable functions, defined by ; the Poisson bracket of two functions on *M* is itself a function on *M*. The Poisson bracket is antisymmetric because:

- .

Furthermore,

.

**(**)

Here *X _{g}f* denotes the vector field

If α is an arbitrary one-form on *M*, the vector field Ω_{α} generates (at least locally) a flow satisfying the boundary condition and the first-order differential equation

The will be symplectomorphisms (canonical transformations) for every *t* as a function of *x* if and only if ; when this is true, Ω_{α} is called a symplectic vector field. Recalling Cartan's identity and *d*ω = 0, it follows that . Therefore Ω_{α} is a symplectic vector field if and only if α is a closed form. Since , it follows that every Hamiltonian vector field *X _{f}* is a symplectic vector field, and that the Hamiltonian flow consists of canonical transformations. From

This is a fundamental result in Hamiltonian mechanics, governing the time evolution of functions defined on phase space. As noted above, when *{f,H} = 0*, *f* is a constant of motion of the system. In addition, in canonical coordinates (with and ), Hamilton's equations for the time evolution of the system follow immediately from this formula.

It also follows from **(1)** that the Poisson bracket is a derivation; that is, it satisfies a non-commutative version of Leibniz's product rule:

, and

**(**)

The Poisson bracket is intimately connected to the Lie bracket of the Hamiltonian vector fields. Because the Lie derivative is a derivation,

- .

Thus if *v* and *w* are symplectic, using , Cartan's identity, and the fact that is a closed form,

It follows that , so that

.

**(**)

Thus, the Poisson bracket on functions corresponds to the Lie bracket of the associated Hamiltonian vector fields. We have also shown that the Lie bracket of two symplectic vector fields is a Hamiltonian vector field and hence is also symplectic. In the language of abstract algebra, the symplectic vector fields form a subalgebra of the Lie algebra of smooth vector fields on *M*, and the Hamiltonian vector fields form an ideal of this subalgebra. The sympletic vector fields are the Lie algebra of the (infinite-dimensional) Lie group of symplectomorphisms of *M*.

It is widely asserted that the Jacobi identity for the Poisson bracket,

follows from the corresponding identity for the Lie bracket of vector fields, but this is true only up to a locally constant function. However, to prove the Jacobi identity for the Poisson bracket, it is sufficient to show that:

where the operator on smooth functions on *M* is defined by and the bracket on the right-hand side is the commutator of operators, . By **(1)**, the operator is equal to the operator *X _{g}*. The proof of the Jacobi identity follows from

The algebra of smooth functions on M, together with the Poisson bracket forms a Poisson algebra, because it is a Lie algebra under the Poisson bracket, which additionally satisfies Leibniz's rule **(2)**. We have shown that every symplectic manifold is a Poisson manifold, that is a manifold with a "curly-bracket" operator on smooth functions such that the smooth functions form a Poisson algebra. However, not every Poisson manifold arises in this way, because Poisson manifolds allow for degeneracy which cannot arise in the symplectic case.

Given a smooth vector field *X* on the configuration space, let *P _{X}* be its conjugate momentum. The conjugate momentum mapping is a Lie algebra anti-homomorphism from the Poisson bracket to the Lie bracket:

This important result is worth a short proof. Write a vector field *X* at point *q* in the configuration space as

where the is the local coordinate frame. The conjugate momentum to *X* has the expression

where the *p _{i}* are the momentum functions conjugate to the coordinates. One then has, for a point

The above holds for all *(q,p)*, giving the desired result.

Poisson brackets deform to Moyal brackets upon quantization, that is, they generalize to a different Lie algebra, the Moyal algebra, or, equivalently in Hilbert space, quantum commutators. The Wigner-İnönü group contraction of these (the classical limit, *ħ*→0) yields the above Lie algebra.

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*Mathematical Methods of Classical Mechanics*(2nd ed.). New York: Springer. ISBN 978-0-387-96890-2.

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*Mechanics*. Course of Theoretical Physics. Vol. 1 (3rd ed.). Butterworth-Heinemann. ISBN 978-0-7506-2896-9.

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