Geometric phase

Berry phase in quantum mechanics

In a quantum system at the n-th eigenstate, an adiabatic evolution of the Hamiltonian sees the system remain in the n-th eigenstate of the Hamiltonian, while also obtaining a phase factor. The phase obtained has a contribution from the state's time evolution and another from the variation of the eigenstate with the changing Hamiltonian. The second term corresponds to the Berry phase and for non-cyclical variations of the Hamiltonian it can be made to vanish by a different choice of the phase associated with the eigenstates of the Hamiltonian at each point in the evolution.

However, if the variation is cyclical, the Berry phase cannot be cancelled, it is invariant and becomes an observable property of the system. From the Schrödinger equation the Berry phase γ can be calculated to be:

γ [ C ] = i ∮ C ⟨ n , t | ( ∇ R | n , t ⟩ ) d R

where R parametrizes the cyclic adiabatic process. It follows a closed path C in the appropriate parameter space. A recent review on the geometric phase effects on electronic properties was given by Xiao, Chang and Niu. Geometric phase along the closed path C can also be calculated by integrating the Berry curvature over surface enclosed by C .

The Foucault pendulum

One of the easiest examples is the Foucault pendulum. An easy explanation in terms of geometric phases is given by von Bergmann and von Bergmann:

How does the pendulum precess when it is taken around a general path C? For transport along the equator, the pendulum will not precess. [...] Now if C is made up of geodesic segments, the precession will all come from the angles where the segments of the geodesics meet; the total precession is equal to the net deficit angle which in turn equals the solid angle enclosed by C modulo 2π. Finally, we can approximate any loop by a sequence of geodesic segments, so the most general result (on or off the surface of the sphere) is that the net precession is equal to the enclosed solid angle.

To put it in different words, there are no inertial forces that could make the pendulum precess, so the precession (relative to the direction of motion of the path along which the pendulum is carried) is entirely due to the turning of this path. Thus the orientation of the pendulum undergoes parallel transport. For the original Foucault pendulum, the path is a circle of latitude, and by the Gauss–Bonnet theorem, the phase shift is given by the enclosed solid angle.

Polarized light in an optical fiber

A second example is linearly polarized light entering a single-mode optical fiber. Suppose the fiber traces out some path in space and the light exits the fiber in the same direction as it entered. Then compare the initial and final polarizations. In semiclassical approximation the fiber functions as a waveguide and the momentum of the light is at all times tangent to the fiber. The polarization can be thought of as an orientation perpendicular to the momentum. As the fiber traces out its path, the momentum vector of the light traces out a path on the sphere in momentum space. The path is closed since initial and final directions of the light coincide, and the polarization is a vector tangent to the sphere. Going to momentum space is equivalent to taking the Gauss map. There are no forces that could make the polarization turn, just the constraint to remain tangent to the sphere. Thus the polarization undergoes parallel transport and the phase shift is given by the enclosed solid angle (times the spin, which in case of light is 1).

Stochastic pump effect

A stochastic pump is a classical stochastic system that responds with nonzero, on average, currents to periodic changes of parameters. The stochastic pump effect can be interpreted in terms of a geometric phase in evolution of the moment generating function of stochastic currents.

Spin ½

The geometric phase can be evaluated exactly for a spin-½ particle in a magnetic field.

Geometric phase defined on attractors

While Berry's formulation was originally defined for linear Hamiltonian systems, it was soon realized by Ning and Haken that similar geometric phase can be defined for entirely different systems such as nonlinear dissipative systems that possess certain cyclic attractors. They showed that such cyclic attractors exist in a class of nonlinear dissipative systems with certain symmetries.

Exposure in molecular adiabatic potential surface intersections

There are several ways to compute the geometric phase in molecules within the Born Oppenheimer framework. One way is through the "non-adiabatic coupling M × M matrix" defined by

τ i j μ = ⟨ ψ i | ∂ μ ψ j ⟩

where ψ i is the adiabatic electronic wave function, depending on the nuclear parameters R μ . The nonadiabatic coupling can be used to define a loop integral, analogous to a Wilson loop (1974) in field theory, developed independently for molecular framework by M. Baer (1975, 1980, 2000). Given a closed loop Γ , parameterized by R μ ( t ) where t ∈ [ 0 , 1 ] is a parameter and R μ ( t + 1 ) = R μ ( t ) . The D-matrix is given by:

D [ Γ ] = P ^ e ∮ Γ τ μ d R μ

(here, P ^ is a path ordering symbol). It can be shown that once M is large enough (i.e. a sufficient number of electronic states is considered) this matrix is diagonal with the diagonal elements equal to e i β j where β j are the geometric phases associated with the loop for the j adiabatic electronic state.

For time-reversal symmetrical electronic Hamiltonians the geometric phase reflects the number of conical intersections encircled by the loop. More accurately:

e i β j = ( − 1 ) N j

where N j is the number of conical intersections involving the adiabatic state ψ j encircled by the loop Γ .

An alternative to the D-matrix approach would be a direct calculation of the Pancharatnam phase. This is especially useful if one is interested only in the geometric phases of a single adiabatic state. In this approach, one takes a number N + 1 of points ( n = 0 , . . . , N ) along the loop R ( t n ) with t 0 = 0 and t N = 1 then using only the jth adiabatic states ψ j [ R ( t n ) ] computes the Pancharatnam product of overlaps:

I j ( Γ , N ) = ∏ n = 0 N − 1 ⟨ ψ j [ R ( t n ) ] | ψ j [ R ( t n + 1 ) ] ⟩

In the limit N → ∞ one has (See Ryb & Baer 2004 for explanation and some applications):

I j ( Γ , N ) → e i β j

Geometric phase and quantization of cyclotron motion

Electron subjected to magnetic field B moves on a circular (cyclotron) orbit.^[1] Classically, any cyclotron radius R c is acceptable. Quantum-mechanically, only discrete energy levels (Landau levels) are allowed and since R c is related to electron's energy, this corresponds to quantized values of R c . The energy quantization condition obtained by solving Schrödinger's equation reads, for example, E = ( n + α ) ℏ ω c , α = 1 / 2 for free electrons (in vacuum) or E = v 2 ( n + α ) e B ℏ , α = 0 for electrons in graphene where n = 0 , 1 , 2 , … .^[2] Although the derivation of these results is not difficult, there is an alternative way of deriving them which offers in some respect better physical insight into the Landau level quantization. This alternative way is based on the semiclassical Bohr-Sommerfeld quantization condition

ℏ ∮ d r ⋅ k − e ∮ d r ⋅ A + ℏ γ = 2 π ℏ ( n + 1 / 2 )

which includes the geometric phase γ picked up by the electron while it executes its (real-space) motion along the closed loop of the cyclotron orbit. For free electrons, γ = 0 while γ = π for electrons in graphene. It turns out that the geometric phase is directly linked to α = 1 / 2 of free electrons and α = 0 of electrons in graphene.