Heisenberg picture

Formulation of quantum mechanics

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i ℏ d d t | Ψ ⟩ = H ^ | Ψ ⟩ {\displaystyle i\hbar {\frac {d}{dt}}|\Psi \rangle ={\hat {H}}|\Psi \rangle }

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In physics, the Heisenberg picture or Heisenberg representation[1] is a formulation (largely due to Werner Heisenberg in 1925) of quantum mechanics in which the operators (observables and others) incorporate a dependency on time, but the state vectors are time-independent, an arbitrary fixed basis rigidly underlying the theory.

It stands in contrast to the Schrödinger picture in which the operators are constant and the states evolve in time. The two pictures only differ by a basis change with respect to time-dependency, which corresponds to the difference between active and passive transformations. The Heisenberg picture is the formulation of matrix mechanics in an arbitrary basis, in which the Hamiltonian is not necessarily diagonal.

It further serves to define a third, hybrid, picture, the interaction picture.

## Mathematical details

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In the Heisenberg picture of quantum mechanics the state vectors |ψ⟩ do not change with time, while observables A satisfy

d d t A H ( t ) = i ℏ [ H H ( t ) , A H ( t ) ] + ( ∂ A S ∂ t ) H , {\displaystyle {\frac {d}{dt}}A_{\text{H}}(t)={\frac {i}{\hbar }}[H_{\text{H}}(t),A_{\text{H}}(t)]+\left({\frac {\partial A_{\text{S}}}{\partial t}}\right)_{\text{H}},}

where "H" and "S" label observables in Heisenberg and Schrödinger picture respectively, H is the Hamiltonian and [·,·] denotes the commutator of two operators (in this case H and A). Taking expectation values automatically yields the Ehrenfest theorem, featured in the correspondence principle.

By the Stone–von Neumann theorem, the Heisenberg picture and the Schrödinger picture are unitarily equivalent, just a basis change in Hilbert space. In some sense, the Heisenberg picture is more natural and convenient than the equivalent Schrödinger picture, especially for relativistic theories. Lorentz invariance is manifest in the Heisenberg picture, since the state vectors do not single out the time or space.

This approach also has a more direct similarity to classical physics: by simply replacing the commutator above by the Poisson bracket, the Heisenberg equation reduces to an equation in Hamiltonian mechanics.

## Equivalence of Heisenberg's equation to the Schrödinger equation

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For the sake of pedagogy, the Heisenberg picture is introduced here from the subsequent, but more familiar, Schrödinger picture.

According to Schrödinger's equation, the quantum state at time  t {\displaystyle t} is  | ψ ( t ) ⟩ = U ( t ) | ψ ( 0 ) ⟩ {\displaystyle |\psi (t)\rangle =U(t)|\psi (0)\rangle } , where  U ( t ) = T e − i ℏ ∫ 0 t d s H S ( s ) {\displaystyle U(t)=Te^{-{\frac {i}{\hbar }}\int _{0}^{t}dsH_{\rm {S}}(s)}} is the time-evolution operator induced by a Hamiltonian  H S ( t ) {\displaystyle H_{\rm {S}}(t)} that could depend on time, and  | ψ ( 0 ) ⟩ {\displaystyle |\psi (0)\rangle } is the initial state.  T {\displaystyle T} refers to time-ordering, ħ is the reduced Planck constant, and i is the imaginary unit. The expectation value of an observable  A S ( t ) {\displaystyle A_{\rm {S}}(t)} in the Schrödinger picture, which is a Hermitian linear operator that could also be time-dependent, in the state  | ψ ( t ) ⟩ {\displaystyle |\psi (t)\rangle } is given by  ⟨ A ⟩ t = ⟨ ψ ( t ) | A S ( t ) | ψ ( t ) ⟩ . {\displaystyle \langle A\rangle _{t}=\langle \psi (t)|A_{\rm {S}}(t)|\psi (t)\rangle .}

In the Heisenberg picture, the quantum state is assumed to remain constant at its initial value  | ψ ( 0 ) ⟩ {\displaystyle |\psi (0)\rangle } , whereas operators evolve with time according to the definition  A H ( t ) := U † ( t ) A S ( t ) U ( t ) . {\displaystyle A_{\rm {H}}(t):=U^{\dagger }(t)A_{\rm {S}}(t)U(t)\,.} This readily implies  ⟨ A ⟩ t = ⟨ ψ ( 0 ) | A H ( t ) | ψ ( 0 ) ⟩ {\displaystyle \langle A\rangle _{t}=\langle \psi (0)|A_{\rm {H}}(t)|\psi (0)\rangle } , so the same expectation value can be obtained by working in either picture. The Schrödinger equation for the time-evolution operator is  d d t U ( t ) = − i ℏ H S ( t ) U ( t ) . {\displaystyle {\frac {d}{dt}}U(t)=-{\frac {i}{\hbar }}H_{\rm {S}}(t)U(t).} It follows that  d d t A H ( t ) = ( d d t U † ( t ) ) A S ( t ) U ( t ) + U † ( t ) A S ( t ) ( d d t U ( t ) ) + U † ( t ) ( ∂ A S ∂ t ) U ( t ) = i ℏ U † ( t ) H S ( t ) A S ( t ) U ( t ) − i ℏ U † ( t ) A S ( t ) H S ( t ) U ( t ) + U † ( t ) ( ∂ A S ∂ t ) U ( t ) = i ℏ U † ( t ) H S ( t ) U ( t ) U † ( t ) A S ( t ) U ( t ) − i ℏ U † ( t ) A S ( t ) U ( t ) U † ( t ) H S ( t ) U ( t ) + ( ∂ A S ∂ t ) H = i ℏ [ H H ( t ) , A H ( t ) ] + ( ∂ A S ∂ t ) H , {\displaystyle {\begin{aligned}{\frac {d}{dt}}A_{\rm {H}}(t)&=\left({\frac {d}{dt}}U^{\dagger }(t)\right)A_{\rm {S}}(t)U(t)+U^{\dagger }(t)A_{\rm {S}}(t)\left({\frac {d}{dt}}U(t)\right)+U^{\dagger }(t)\left({\frac {\partial A_{\rm {S}}}{\partial t}}\right)U(t)\\\&={\frac {i}{\hbar }}U^{\dagger }(t)H_{\rm {S}}(t)A_{\rm {S}}(t)U(t)-{\frac {i}{\hbar }}U^{\dagger }(t)A_{\rm {S}}(t)H_{\rm {S}}(t)U(t)+U^{\dagger }(t)\left({\frac {\partial A_{\rm {S}}}{\partial t}}\right)U(t)\\\&={\frac {i}{\hbar }}U^{\dagger }(t)H_{\rm {S}}(t)U(t)U^{\dagger }(t)A_{\rm {S}}(t)U(t)-{\frac {i}{\hbar }}U^{\dagger }(t)A_{\rm {S}}(t)U(t)U^{\dagger }(t)H_{\rm {S}}(t)U(t)+\left({\frac {\partial A_{\rm {S}}}{\partial t}}\right)_{\rm {H}}\\\&={\frac {i}{\hbar }}[H_{\rm {H}}(t),A_{\rm {H}}(t)]+\left({\frac {\partial A_{\rm {S}}}{\partial t}}\right)_{\rm {H}},\end{aligned}}} where differentiation was carried out according to the product rule. This is Heisenberg's equation of motion. Note that the Hamiltonian that appears in the final line above is the Heisenberg Hamiltonian  H H ( t ) {\displaystyle H_{\rm {H}}(t)} , which may differ from the Schrödinger Hamiltonian  H S ( t ) {\displaystyle H_{\rm {S}}(t)} .

An important special case of the equation above is obtained if the Hamiltonian H S {\displaystyle H_{\rm {S}}} does not vary with time. Then the time-evolution operator can be written as  U ( t ) = e − i ℏ t H S , {\displaystyle U(t)=e^{-{\frac {i}{\hbar }}tH_{\rm {S}}},} and hence  H H ≡ H S ≡ H {\displaystyle H_{\rm {H}}\equiv H_{\rm {S}}\equiv H} since  U ( t ) {\displaystyle U(t)} now commutes with  H {\displaystyle H} . Therefore,  ⟨ A ⟩ t = ⟨ ψ ( 0 ) | e i ℏ t H A S ( t ) e − i ℏ t H | ψ ( 0 ) ⟩ {\displaystyle \langle A\rangle _{t}=\langle \psi (0)|e^{{\frac {i}{\hbar }}tH}A_{\rm {S}}(t)e^{-{\frac {i}{\hbar }}tH}|\psi (0)\rangle } and following the previous analyses,  d d t A H ( t ) = i ℏ [ H , A H ( t ) ] + e i ℏ t H ( ∂ A S ∂ t ) e − i ℏ t H . {\displaystyle {\begin{aligned}{\frac {d}{dt}}A_{\rm {H}}(t)&={\frac {i}{\hbar }}[H,A_{\rm {H}}(t)]+e^{{\frac {i}{\hbar }}tH}\left({\frac {\partial A_{\rm {S}}}{\partial t}}\right)e^{-{\frac {i}{\hbar }}tH}.\end{aligned}}}

Furthermore, if  A S ≡ A {\displaystyle A_{\rm {S}}\equiv A} is also time-independent, then the last term vanishes and

d d t A H ( t ) = i ℏ [ H , A H ( t ) ] , {\displaystyle {\frac {d}{dt}}A_{\rm {H}}(t)={\frac {i}{\hbar }}[H,A_{\rm {H}}(t)],}

where  A H ( t ) ≡ A ( t ) = e i ℏ t H A e − i ℏ t H {\displaystyle A_{\rm {H}}(t)\equiv A(t)=e^{{\frac {i}{\hbar }}tH}Ae^{-{\frac {i}{\hbar }}tH}} in this particular case. The equation is solved by use of the standard operator identity, e B A e − B = A + [ B , A ] + 1 2 ! [ B , [ B , A ] ] + 1 3 ! [ B , [ B , [ B , A ] ] ] + ⋯ , {\displaystyle {e^{B}Ae^{-B}}=A+[B,A]+{\frac {1}{2!}}[B,[B,A]]+{\frac {1}{3!}}[B,[B,[B,A]]]+\cdots \,,} which implies  A ( t ) = A + i t ℏ [ H , A ] + 1 2 ! ( i t ℏ ) 2 [ H , [ H , A ] ] + 1 3 ! ( i t ℏ ) 3 [ H , [ H , [ H , A ] ] ] + ⋯ {\displaystyle A(t)=A+{\frac {it}{\hbar }}[H,A]+{\frac {1}{2!}}\left({\frac {it}{\hbar }}\right)^{2}[H,[H,A]]+{\frac {1}{3!}}\left({\frac {it}{\hbar }}\right)^{3}[H,[H,[H,A]]]+\cdots }

A similar relation also holds for classical mechanics, the classical limit of the above, given by the correspondence between Poisson brackets and commutators:  [ A , H ] ⟷ i ℏ { A , H } . {\displaystyle [A,H]\quad \longleftrightarrow \quad i\hbar \\{A,H\\}.} In classical mechanics, for an A with no explicit time dependence,  { A , H } = d A d t , {\displaystyle \\{A,H\\}={\frac {dA}{dt}}~,} so again the expression for A(t) is the Taylor expansion around t = 0.

In effect, the initial state of the quantum system has receded from view, and is only considered at the final step of taking specific expectation values or matrix elements of observables that evolved in time according to the Heisenberg equation of motion. A similar analysis applies if the initial state is mixed.

The time evolved state  | ψ ( t ) ⟩ {\displaystyle |\psi (t)\rangle } in the Schrödinger picture is sometimes written as  | ψ S ( t ) ⟩ {\displaystyle |\psi _{\rm {S}}(t)\rangle } to differentiate it from the evolved state  | ψ I ( t ) ⟩ {\displaystyle |\psi _{\rm {I}}(t)\rangle } that appears in the different interaction picture.

## Commutator relations

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Commutator relations may look different than in the Schrödinger picture, because of the time dependence of operators. For example, consider the operators x(t1), x(t2), p(t1) and p(t2). The time evolution of those operators depends on the Hamiltonian of the system. Considering the one-dimensional harmonic oscillator,  H = p 2 2 m + m ω 2 x 2 2 , {\displaystyle H={\frac {p^{2}}{2m}}+{\frac {m\omega ^{2}x^{2}}{2}},} the evolution of the position and momentum operators is given by:  d d t x ( t ) = i ℏ [ H , x ( t ) ] = p m , {\displaystyle {\frac {d}{dt}}x(t)={\frac {i}{\hbar }}[H,x(t)]={\frac {p}{m}},} d d t p ( t ) = i ℏ [ H , p ( t ) ] = − m ω 2 x . {\displaystyle {\frac {d}{dt}}p(t)={\frac {i}{\hbar }}[H,p(t)]=-m\omega ^{2}x.}

Note that the Hamiltonian is time independent and hence  x ( t ) , p ( t ) {\displaystyle x(t),p(t)} are the position and momentum operators in the Heisenberg picture. Differentiating both equations once more and solving for them with proper initial conditions,  p ˙ ( 0 ) = − m ω 2 x 0 , {\displaystyle {\dot {p}}(0)=-m\omega ^{2}x_{0},} x ˙ ( 0 ) = p 0 m , {\displaystyle {\dot {x}}(0)={\frac {p_{0}}{m}},} leads to  x ( t ) = x 0 cos ⁡ ( ω t ) + p 0 ω m sin ⁡ ( ω t ) , {\displaystyle x(t)=x_{0}\cos(\omega t)+{\frac {p_{0}}{\omega m}}\sin(\omega t),} p ( t ) = p 0 cos ⁡ ( ω t ) − m ω x 0 sin ⁡ ( ω t ) . {\displaystyle p(t)=p_{0}\cos(\omega t)-m\omega x_{0}\sin(\omega t).}

Direct computation yields the more general commutator relations,  [ x ( t 1 ) , x ( t 2 ) ] = i ℏ m ω sin ⁡ ( ω t 2 − ω t 1 ) , {\displaystyle [x(t_{1}),x(t_{2})]={\frac {i\hbar }{m\omega }}\sin \left(\omega t_{2}-\omega t_{1}\right),} [ p ( t 1 ) , p ( t 2 ) ] = i ℏ m ω sin ⁡ ( ω t 2 − ω t 1 ) , {\displaystyle [p(t_{1}),p(t_{2})]=i\hbar m\omega \sin \left(\omega t_{2}-\omega t_{1}\right),} [ x ( t 1 ) , p ( t 2 ) ] = i ℏ cos ⁡ ( ω t 2 − ω t 1 ) . {\displaystyle [x(t_{1}),p(t_{2})]=i\hbar \cos \left(\omega t_{2}-\omega t_{1}\right).}

For  t 1 = t 2 {\displaystyle t_{1}=t_{2}} , one simply recovers the standard canonical commutation relations valid in all pictures.

## Summary comparison of evolution in all pictures

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For a time-independent Hamiltonian HS, where H0,S is the free Hamiltonian,

Evolution of:  | Picture (

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Schrödinger (S)  | Heisenberg (H)  | Interaction (I)
Ket state |  | ψ S ( t ) ⟩ = e − i H S t / ℏ | ψ S ( 0 ) ⟩ {\displaystyle |\psi _{\rm {S}}(t)\rangle =e^{-iH_{\rm {S}}~t/\hbar }|\psi _{\rm {S}}(0)\rangle } | constant  |  | ψ I ( t ) ⟩ = e i H 0 , S t / ℏ | ψ S ( t ) ⟩ {\displaystyle |\psi _{\rm {I}}(t)\rangle =e^{iH_{0,\mathrm {S} }~t/\hbar }|\psi _{\rm {S}}(t)\rangle }
Observable | constant  |  A H ( t ) = e i H S t / ℏ A S e − i H S t / ℏ {\displaystyle A_{\rm {H}}(t)=e^{iH_{\rm {S}}~t/\hbar }A_{\rm {S}}e^{-iH_{\rm {S}}~t/\hbar }} |  A I ( t ) = e i H 0 , S t / ℏ A S e − i H 0 , S t / ℏ {\displaystyle A_{\rm {I}}(t)=e^{iH_{0,\mathrm {S} }~t/\hbar }A_{\rm {S}}e^{-iH_{0,\mathrm {S} }~t/\hbar }}
Density matrix |  ρ S ( t ) = e − i H S t / ℏ ρ S ( 0 ) e i H S t / ℏ {\displaystyle \rho _{\rm {S}}(t)=e^{-iH_{\rm {S}}~t/\hbar }\rho _{\rm {S}}(0)e^{iH_{\rm {S}}~t/\hbar }} | constant  |  ρ I ( t ) = e i H 0 , S t / ℏ ρ S ( t ) e − i H 0 , S t / ℏ {\displaystyle \rho _{\rm {I}}(t)=e^{iH_{0,\mathrm {S} }~t/\hbar }\rho _{\rm {S}}(t)e^{-iH_{0,\mathrm {S} }~t/\hbar }}

## See also

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* Bra–ket notation
* Interaction picture
* Schrödinger picture
* Heisenberg–Langevin equations
* Phase space formulation

## References

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1. ^ "Heisenberg representation". Encyclopedia of Mathematics. Retrieved 3 September 2013.

* Cohen-Tannoudji, Claude; Bernard Diu; Frank Laloe (1977). Quantum Mechanics (Volume One). Paris: Wiley. pp. 312–314. ISBN 0-471-16433-X.
* Albert Messiah, 1966. Quantum Mechanics (Vol. I), English translation from French by G. M. Temmer. North Holland, John Wiley & Sons.
* Merzbacher E., Quantum Mechanics (3rd ed., John Wiley 1998) pp. 430–431 ISBN 0-471-88702-1
* L.D. Landau, E.M. Lifshitz (1977). Quantum Mechanics: Non-Relativistic Theory. Vol. 3 (3rd ed.). Pergamon Press. ISBN 978-0-08-020940-1. Online copy
* R. Shankar (1994); Principles of Quantum Mechanics, Plenum Press, ISBN 978-0306447907.
* J. J. Sakurai (1993); Modern Quantum Mechanics (Revised Edition), ISBN 978-0201539295.

## External links

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* Pedagogic Aides to Quantum Field Theory Click on the link for Chap. 2 to find an extensive, simplified introduction to the Heisenberg picture.
* Some expanded derivations and an example of the harmonic oscillator in the Heisenberg picture [1]
* The original Heisenberg paper translated (although difficult to read, it contains an example for the anharmonic oscillator): Sources of Quantum mechanics B.L. Van Der Waerden [2]
* The computations for the hydrogen atom in the Heisenberg representation originally from a paper of Pauli [3]

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Quantum mechanics

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* Born rule
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