Superradiant phase transition

In quantum optics, a superradiant phase transition is a phase transition that occurs in a collection of fluorescent emitters (such as atoms), between a state containing few electromagnetic excitations (as in the electromagnetic vacuum) and a superradiant state with many electromagnetic excitations trapped inside the emitters. The superradiant state is made thermodynamically favorable by having strong, coherent interactions between the emitters.

The superradiant phase transition was originally predicted by the Dicke model of superradiance which assumes that atoms have only two energetic levels, which interact with only one mode of the electromagnetic field. ^[1] ^[2] The phase transition occurs when the strength of the interaction between the atoms and the field is greater than the energy of the non-interacting part of the system. (This is similar to the case of superconductivity in ferromagnetism, which leads to the dynamic interaction between ferromagnetic atoms and the spontaneous ordering of excitations below the critical temperature). The collective Lamb shift, relating to the system of atoms interacting with the vacuum fluctuations, becomes comparable to the energies of atoms alone, and the vacuum fluctuations cause the spontaneous self-excitation of matter.

The transition can be readily understood by the use of the Holstein-Primakoff transformation^[3] applied to a two level atom. As a result of this transformation, the atoms become Lorentz harmonic oscillators with frequencies equal to the difference between the energy levels. The whole system then simplifies to a system of interacting harmonic oscillators of atoms, and the field known as Hopfield dielectric which further predicts in the normal state polarons for photons or polaritons. If the interaction with the field is so strong that the system collapses in the harmonic approximation and complex polariton frequencies (soft modes) appear, then the physical system with nonlinear terms of the higher order becomes the system with the Mexican hat-like potential, and will undergo ferroelectric-like phase transition.^[4] In this model, the system is mathematically equivalent for one mode of excitation to the Trojan wave packet when the circularly polarized field intensity corresponds to the electromagnetic coupling constant. Above the critical value it changes to the unstable motion of the ionization.

The superradiant phase transition was the subject of a wide discussion as to whether or not it is only a result of the simplified model of the matter-field interaction; and if it can occur for the real physical parameters of physical systems (a no-go theorem).^[5]^[6] However, both the original derivation and the later corrections leading to nonexistence of the transition due to Thomas–Reiche–Kuhn sum rule canceling for the harmonic oscillator the needed inequality to impossible negativity of the interaction were based on the assumption that the quantum field operators are commuting numbers, and the atoms do not interact with the static Coulomb forces. This is generally not true. It can be observed in model systems like Bose–Einstein condensates and artificial atoms.^[7]^[8]

Theory

Criticality of linearized Jaynes-Cummings model

A superradiant phase transition is formally predicted by the critical behavior of the resonant Jaynes-Cummings model, describing the interaction of only one atom with one mode of the electromagnetic field. Starting from the exact Hamiltonian of the Jaynes-Cummings model at resonance

{\hat {H}}_{\text{JC}}=\hbar \omega {\hat {a}}^{\dagger }{\hat {a}}+\hbar \omega {\frac {{\hat {\sigma }}_{z}}{2}}+{\frac {\hbar \Omega }{2}}\left({\hat {a}}{\hat {\sigma }}_{+}+{\hat {a}}^{\dagger }{\hat {\sigma }}_{-}+{\hat {a}}{\hat {\sigma }}_{-}+{\hat {a}}^{\dagger }{\hat {\sigma }}_{+}\right),

Applying the Holstein-Primakoff transformation for two spin levels and replacing the spin raising and lowering operators by those for the harmonic oscillators

{\hat {\sigma }}_{-}\approx {\hat {b}}

{\hat {\sigma }}_{+}\approx {\hat {b}}^{\dagger }

{\hat {\sigma }}_{z}\approx 2{\hat {b}}^{\dagger }{\hat {b}}

one gets the Hamiltonian of two coupled harmonic oscillators:

{\hat {H}}_{\text{JC}}=\hbar \omega {\hat {a}}^{\dagger }{\hat {a}}+\hbar \omega {\hat {b}}^{\dagger }{\hat {b}}+{\frac {\hbar \Omega }{2}}\left({\hat {a}}{\hat {b}}^{\dagger }+{\hat {a}}^{\dagger }{\hat {b}}+{\hat {a}}{\hat {b}}+{\hat {a}}^{\dagger }{\hat {b}}^{\dagger }\right),

which readily can be diagonalized. Postulating its normal form

{\hat {H}}_{\text{JC}}=\Omega _{+}{\hat {A_{+}}}^{\dagger }{\hat {A_{+}}}+\Omega _{-}{\hat {A_{-}}}^{\dagger }{\hat {A_{-}}}+C

where

{\hat {A_{\pm }}}=c_{\pm 1}{\hat {a}}+c_{\pm 2}{\hat {a}}^{\dagger }+c_{\pm 3}{\hat {b}}+c_{\pm 4}{\hat {b}}^{\dagger }

one gets the eigenvalue equation

[{\hat {A_{\pm }}},{\hat {H}}_{\text{JC}}]=\Omega _{\pm }A

with the solutions

\Omega _{\pm }=\omega {\sqrt {1\pm {\frac {\Omega }{\omega }}}}

The system collapses when one of the frequencies becomes imaginary i.e. when

\Omega >\omega

or when the atom-field coupling is stronger than the frequency of the mode and atom oscillators. While there are physically higher terms in the true system, the system in this regime will therefore undergo the phase transition.

Criticality of Jaynes-Cummings model

The simplified Hamiltonian of the Jaynes-Cummings model neglecting the counter-rotating terms is

{\hat {H}}_{\text{JC}}=\hbar \omega {\hat {a}}^{\dagger }{\hat {a}}+\hbar \omega {\frac {{\hat {\sigma }}_{z}}{2}}+{\frac {\hbar \Omega }{2}}\left({\hat {a}}{\hat {\sigma }}_{+}+{\hat {a}}^{\dagger }{\hat {\sigma }}_{-}\right),

and the energies for the case of zero detuning are

E_{\pm }(n)=\hbar \omega \left(n+{\frac {1}{2}}\right)\pm {\frac {1}{2}}\hbar \Omega (n),

\Omega (n)=\Omega {\sqrt {n+1}}

where $\Omega _{n}$ is the Rabi frequency. One can approximately calculate the canonical partition function

Z=\sum _{\pm ,n}\mathrm {e} ^{-\beta E_{\pm }(n)}\approx \sum _{\pm }\int \mathrm {e} ^{-\beta E_{\pm }(n)}dn=\int \mathrm {e} ^{\Phi (n)}dn

where the discrete sum was replaced by the integral.

The normal approach is that the later integral is calculated by the Gaussian approximation around the maximum of the exponent:

{\frac {\partial \Phi (n)}{\partial n}}=0

\Phi (n)=-\beta \hbar \omega \left(n+{\frac {1}{2}}\right)+\log 2\cosh {\frac {\hbar \Omega (n)\beta }{2}}

This leads to the critical equation

\tanh {\frac {\hbar \Omega (n)\beta }{2}}=4{\frac {\omega }{\Omega }}{\sqrt {n+1}}

This has the solution only if

\Omega >4\omega

which means that the normal, and the superradiant phase exist only if the field-atom coupling is significantly stronger than the energy difference between the atom levels. When the condition is fulfilled, the equation gives the solution for the order parameter $n$ depending on the inverse of the temperature $1/\beta$ , which means non-vanishing ordered field mode. Similar considerations can be done in true thermodynamic limit of the infinite number of atoms.

References

↑ Hepp, Klaus; Lieb, Elliott H. (1973). "On the superradiant phase transition for Molecules in a Quantized Radiation Field: Dicke Maser Model". Annals of Physics. 76: 360–404. Bibcode:1973AnPhy..76..360H. doi:10.1016/0003-4916(73)90039-0.
↑ Wang, Y. K.; Hioe, F. T (1973). "Phase Transition in the Dicke Model of Superradiance". Physical Review A. 7: 831–836. Bibcode:1973PhRvA...7..831W. doi:10.1103/PhysRevA.7.831.
↑ Baksic, Alexandre; Nataf, Pierre; Ciuti, Cristiano (2013). "Superradiant phase transitions with three-level systems". Physical Review A. 87: 023813–023813–5. arXiv:1212.5080. Bibcode:2013PhRvA..87a3813D. doi:10.1103/PhysRevA.87.013813.
↑ Emaljanov, V. I.; Klimontovicz, Yu. L. (1976). "Appearance of Collective Polarisation as a Result of Phase Transition in an Ensemble of Two-level Atoms Interacting Through Electromagnetic Field". Physics Letters A. 59 (5): 366–368. Bibcode:1976PhLA...59..366E. doi:10.1016/0375-9601(76)90411-4.
↑ Rzążewski, K.; Wódkiewicz, K. T (1975). "Phase Transitions, Two Level Atoms, and the $A^{2}$ Term". Physical Review Letters. 35 (7): 432–434. Bibcode:1975PhRvL..35..432R. doi:10.1103/PhysRevLett.35.432.
↑ Bialynicki-Birula, Iwo; Rzążewski, Kazimierz (1979). "No-go theorem concerning the superradiant phase transition in atomic systems". Physical Review A. 19 (1): 301–303. Bibcode:1979PhRvA..19..301B. doi:10.1103/PhysRevA.19.301.
↑ Zhang, Yuanwei; Lian, Jinling; Liang, J.-Q.; Chen, Gang; Zhang, Chuanwei; Suotang, Jia (2013). "Finite-temperature Dicke phase transition of a Bose-Einstein condensate in an optical cavity". Physical Review A. 87: 013616–013616–6. arXiv:1202.4125. Bibcode:2013PhRvA..87a3616Z. doi:10.1103/PhysRevA.87.013616.
↑ Viehmann, Oliver; von Delft, Jan; Marquard, Florian (1975). "Superradiant Phase Transitions and the Standard Description of Circuit QED". Physical Review Letters. 107 (7): 113602–113602–5. doi:10.1103/physrevlett.107.113602.

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