Gell-Mann and Low theorem

The Gell-Mann and Low theorem is a theorem in quantum field theory that allows one to relate the ground (or vacuum) state of an interacting system to the ground state of the corresponding non-interacting theory. It was proved in 1951 by Murray Gell-Mann and Francis E. Low. The theorem is useful because, among other things, by relating the ground state of the interacting theory to its non-interacting ground state, it allows one to express Green's functions (which are defined as expectation values of Heisenberg-picture fields in the interacting vacuum) as expectation values of interaction picture fields in the non-interacting vacuum. While typically applied to the ground state, the Gell-Mann and Low theorem applies to any eigenstate of the Hamiltonian. Its proof relies on the concept of starting with a non-interacting Hamiltonian and adiabatically switching on the interactions.

History

The theorem was proved first by Gell-Mann and Low in 1951, making use of the Dyson series. In 1969 Klaus Hepp provided an alternative derivation for the case where the original Hamiltonian describes free particles and the interaction is norm bounded. In 1989 Nenciu and Rasche proved it using the adiabatic theorem. A proof that does not rely on the Dyson expansion was given in 2007 by Molinari.

Statement of the theorem

Let |\Psi_0\rangle be an eigenstate of H_0 with energy E_0 and let the 'interacting' Hamiltonian be H=H_0 + gV, where g is a coupling constant and V the interaction term. We define a Hamiltonian H_\epsilon=H_0 + e^{-\epsilon |t|}gV which effectively interpolates between H and H_0 in the limit \epsilon \rightarrow 0^+ and |t|\rightarrow\infty. Let U_{\epsilon I} denote the evolution operator in the interaction picture. The Gell-Mann and Low theorem asserts that if the limit as \epsilon\rightarrow 0^+ of

 |\Psi^{(\pm)}_\epsilon \rangle = \frac{ U_{\epsilon I} (0,\pm\infty)  |\Psi_0 \rangle}{\langle \Psi_0 | U_{\epsilon I}(0,\pm\infty)|\Psi_0\rangle}

exists, then |\Psi^{(\pm)}_\epsilon \rangle are eigenstates of H.

Note that when applied to, say, the ground-state, the theorem does not guarantee that the evolved state will be a ground state. In other words, level crossing is not excluded.

Proof

As in the original paper, the theorem is typically proved making use of Dyson's expansion of the evolution operator. Its validity however extends beyond the scope of perturbation theory as has been demonstrated by Molinari. We follow Molinari's method here. Focus on H_\epsilon and let g=e^{\epsilon \theta}. From Schrödinger's equation for the time-evolution operator

 i\hbar \partial_{t_1} U_\epsilon(t_1,t_2) = H_\epsilon(t_1) U_\epsilon(t_1,t_2)

and the boundary condition that U_\epsilon(t,t)=1 we can formally write


U_\epsilon(t_1,t_2) = 1+ \frac{1}{i\hbar} \int_{t_2}^{t_1} dt' (H_0 + e^{\epsilon(\theta -|t'|)} V) U_\epsilon(t',t_2).

Focus for the moment on the case 0\geq t_2\geq t_1. Through a change of variables we can write


U_\epsilon(t_1,t_2) = 1+ \frac{1}{i\hbar} \int_{\theta +t_2}^{\theta+t_1} dt' (H_0 + e^{\epsilon t'} V) U_\epsilon(t'-\theta,t_2).

We therefore have that


\partial_\theta U_\epsilon(t_1,t_2) = \epsilon g \partial_g U_\epsilon(t_1,t_2) = \partial_{t_1} U_\epsilon(t_1,t_2) + \partial_{t_2} U_\epsilon(t_1,t_2).

This result can be combined with the Schrödinger equation and its adjoint

 -i\hbar \partial_{t_1} U_\epsilon(t_2,t_1) =  U_\epsilon(t_2,t_1) H_\epsilon(t_1)

to obtain


i\hbar \epsilon g \partial_g U_\epsilon(t_1,t_2) = H_\epsilon(t_1)U_\epsilon(t_1,t_2)- U_\epsilon (t_1,t_2)H_\epsilon (t_2).

The corresponding equation between H_{\epsilon I}, U_{\epsilon I} is the same. It can be obtained by pre-multiplying both sides with e^{i H_0 t_1/\hbar}, post-multiplying with e^{i H_0 t_2/\hbar} and making use of


U_{\epsilon I} (t_1,t_2) = e^{i H_0 t_1/\hbar} U_{\epsilon}(t_1,t_2) e^{-i H_0 t_2 /\hbar}.

The other case we are interested in, namely t_2\geq t_1 \geq 0 can be treated in an analogous fashion and yields an additional minus sign in front of the commutator (we are not concerned here with the case where t_{1,2} have mixed signs). In summary, we obtain


\left(H_{\epsilon, t=0}-E_0 \pm i \hbar \epsilon g \partial_g\right) U_{\epsilon I}(0,\pm\infty) |\Psi_0\rangle = 0.

We proceed for the negative-times case. Abbreviating the various operators for clarity

i \hbar \epsilon g \partial_g \left(U|\Psi_0\rangle\right) = (H_\epsilon-E_0)U|\Psi_0\rangle.

Now using the definition of \Psi_\epsilon we differentiate and eliminate derivatives \partial_g(U|\Psi_0\rangle) using the above expression, finding


\begin{align}
i \hbar \epsilon g \partial_g | \Psi_\epsilon \rangle &= 
\frac{1}{\langle\Psi_0| U |\Psi_0 \rangle} (H_\epsilon-E_0) U|\Psi_0\rangle 
- \frac{U|\Psi_0\rangle }{{\langle\Psi_0 |U| \Psi_0 \rangle}^2} \langle \Psi_0 | H_\epsilon-E_0 | \Psi_0\rangle \\

&= (H_\epsilon-E_0)|\Psi_\epsilon\rangle - |\Psi_\epsilon\rangle \langle \Psi_0 |H_\epsilon-E_0|\Psi_\epsilon\rangle \\

& = \left[ H_\epsilon - E \right] |\Psi_\epsilon\rangle.
\end{align}

where E = E_0 + \langle\Psi_0 | H_\epsilon-H_0 | \Psi_\epsilon\rangle. We can now let \epsilon\rightarrow 0^+ as by assumption the g \partial_g | \Psi_\epsilon \rangle in left hand side is finite. We then clearly see that |\Psi_\epsilon\rangle is an eigenstate of H and the proof is complete.

References

1. M. Gell-Mann and F. Low: "Bound States in Quantum Field Theory", Phys. Rev. 84, 350 (1951)

2. K. Hepp: Lecture Notes in Physics (Springer-Verlag, New York, 1969), Vol. 2.

3. G. Nenciu and G. Rasche: "Adiabatic theorem and Gell-Mann-Low formula", Helv. Phys. Acta 62, 372 (1989).

4. L.G. Molinari: "Another proof of Gell-Mann and Low's theorem", J. Math. Phys. 48, 052113 (2007)

5. A.L. Fetter and J.D. Walecka: "Quantum Theory of Many-Particle Systems", McGraw–Hill (1971)

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