Extended Bose-Hubbard Model with Cavity-Mediated Infinite-Range Interactions at Finite Temperatures

We consider the finite-temperature properties of the extended Bose-Hubbard model realized recently in an ETH experiment [Nature 532, 476 (2016)]. Competing short- and global-range interactions accommodate fascinating collective phenomena. We formulate a self-consistent mean-field theory to describe the behaviors of the system at finite temperatures. At a fixed chemical potential, we map out the distributions of the superfluid order parameters and number densities with respect to the temperatures. For a charge density wave, we find that the global-range interaction enhances the charge order by increasing the transition temperature at which the charge order melts out, while for a supersolid phase, we find that the disappearance of the charge order and the superfluid order occurs at different temperature. At a fixed number-density filling factor, we extract the temperature dependence of the thermodynamic functions such as internal energy, specific heat and entropy. Across the superfluid phase transition, the specific heat has a discontinuous jump.

The experimental progress in coupling degenerate quantum gases with light in high-Q cavities [1][2][3][4][5][6][7][8][9] has opened a new avenue for creating and exploring novel many-body collective phenomena [10][11][12] . A paradigmatic example is the experimental realization of the Dicke model with a gas of ultracold quantum gases inside an optical cavity 4,6 , which allows for access to a superradiant phase transition associated with the breaking of a  2 symmetry 13 . In combination with an optical lattice 14 , recent experiment has realized competing short-and long-range interactions 7 between atoms, which accommodates a multitude of novel symmetry-broken phases, such as the charge density wave and supersolid phases. By trapping Bose-Einstein condensates inside the intersection of two high-finesse optical cavities and illuminating them by a transverse pump beam, the ETH group successfully observed supersolid formation breaking a continuous translation symmetry 8,9 . All these exciting experimental achievements have sparked intense theoretical efforts [15][16][17][18][19][20][21][22][23] concerning novel collective phenomena and dissipative dynamics arising from the cavity-mediated interactions. In particular, the extended Bose-Hubbard model realized in ETH experiment 7,24,25 has attracted much theoretical attention. The model consists of a variation of the standard two-dimensional Bose-Hubbard model [26][27][28][29] that includes a global-range interaction between atoms in the different checkerboard sublattices of a square lattice. It presents in total four quantum phases: superfluid (SF), supersolid (SS), Mott insulator (MI), and charge density wave (CDW). Previous theoretical studies [30][31][32][33][34][35][36][37][38] mainly concentrate on the ground-state phase diagram and associated phase transitions of the model, leaving the finite-temperature physics which is experimentally relevant and interesting, largely intact.
In this work, we shall carry out a self-consistent mean-field study on the finite-temperature properties of the system, with the aim of providing qualitative predictions for future experimental investigation, as understanding even the finite-temperature properties of the conventional Bose-Hubbard model at quantitative level is a nontrivial task [39][40][41][42][43][44][45] . The paper is structured as follows: In Sec. II, the model is introduced and the theoretical formalism is developed. In Sec. III, we present relevant calculation results. Finally, in Sec. IV, the conclusions are drawn.
To decouple the kinetic part of the Hamiltonian, we follow the usual procedures 46 of introducing superfluid order parameters ψ =b i i , resulting in a mean-field Hamiltonian for a supercell (with one even site and one odd site): where the coordination number is z = 2d with d being the dimension of the system, h.c. stands for a hermitian conjugate, and subindex e and o denotes even site and odd site, respectively.
We may diagonalize Ĥ MF in the occupation number space spanned with

calculation and Results
Before embarking on a detailed study on finite-temperature properties of the system, we consider the system at zero temperature and at the atomic limit where zJ/U = 0. Since the superfluid order parameters vanish in this case, the mean-field Hamiltonian reduces tôˆˆˆˆ∑ Minimizing the eigenvalue ε(n e , n o ), one obtains the ground-state phase diagram at the atomic limit. We show the phase diagram in Fig. 1 for the parameter regime K/U ∈ [0, 1/2]. It features two types of incompressible phases: Mott insulating phases (MI) and charge density wave phases (CDW). The Mott phase MI (ne, no) is characterized by equal population on even site and odd site with n e = n o , while the CDW (ne, no) phase is characterized by unequal population on even site and odd site with n e ≠ n o . We may always assume that n e ≥ n o as the system enjoys a  2 symmetry.
The effects of finite temperatures on a charge density wave is shown in Fig. 2. In panel (a) where K/U = 0.2, at zero temperature the system is in the CDW (2,1) phase. As the temperature goes up, the density on even site n e decreases from an integer value, while the density on odd site n o increases. There exists a critical temperature at which the density on both sites become equal with n e = n o , indicating that the charge order parameter Θ vanishes. During the process, we have kept the chemical potential to be fixed at μ/U = 1.0, and the total density n = n e + n o is almost a constant. In panel (b) where K/U = 0.3, the trend is similar as in panel (a), except that the critical temperature above which the charge order becomes zero increases from 10 U/k B to approximately 0.15 U/k B . This fact suggests that for a CDW phase increasing the global-range interaction strength enhances the charge order by increasing the critical temperature.
Now we take the effects of a finite hopping amplitude into account as well. At sufficient magnitude of hopping parameter zJ/U, one expects that the system possesses superfluidity with a nonzero order parameter ψ. We show the behaviors of the order parameter ψ as a function of varying temperatures k B T/U for different hopping parameters zJ/U in Fig. 3. At zero temperature and μ/U = 1.5, the system is in the phase of MI (2,2) with a vanishing charge order, as can be read from Fig. 1. Now a sufficiently large hopping amplitude (zJ/U = 0.15) gives rise to a homogeneous superfluid state with ψ e = ψ o . As the temperature increases, the superfluid order parameter decreases gradually, and eventually the superfluid order parameter ψ e vanishes above the transition temperature T c . It is evident that a larger hopping amplitude leads to a larger transition temperature. When the magnitude of the global-range interaction is changed to K/U = 0.3, our numerical results doesn't get modified. This is expected as the effective Hamiltonian in Eq. (3) for Θ = 0 reduces to two decoupled conventional Bose-Hubbard models at even and odd sites. We proceed to consider the effects of finite temperatures on the supersolid phase, where both superfluid order and charge order are present. As shown in Fig. 4(a), with the increasing of the temperature, both the superfluid order parameter ψ e and ψ o decrease. When the temperature reaches a certain value, the system becomes a conventional superfluid with ψ e = ψ o . As the temperature is increased further to T c1 , the system enters into a CDW state with vanishing superfluid order parameter. Meanwhile, the number densities at both sites display striking behaviors in Fig. 4(b). The number density n e decreases as the temperature goes up, while the number density n o increases correspondingly, demonstrating that the transferring of the particles from sites of high population to sites of low population due to the increasing of temperature. At the temperature rises to the superfluid transition temperature T c1 , there still exists some residual charge order, which is destroyed completely only after the temperature is lifted to a higher critical temperature T c2 .
We turn our attention to the thermodynamics of the system at a fixed filling factor f = (n e + n o )/2. We shall follow the sequences as we study the temperature dependence of the superfluid order parameters and number densities. For the charge density discussed in Fig. 2, its thermodynamic functions such as energy, specific heat, entropy and chemical potential are shown in Fig. 5. The energy per particle E/NU increases steadily with the temperature k B T/U. It is remarkable that a larger global-range interaction K/U leads to a lower energy below the transition temperature. At the transition point where the charge order is completely melted, the specific heat C V /Nk B shows a characteristic cusp. The entropy per particle S/Nk B starting from zero increases monotonically with the temperature, a sign of increasing disorder. Interestingly, the chemical potential decreases slightly with increasing temperatures and does not depend on the strength of global-range interaction. When the temperature is sufficiently high, the thermodynamics of the system is immune to the strength of global-range interaction K/U.
We continue to consider the thermodynamics of conventional superfluid state. The temperature dependence of relevant order parameters is revealed in Fig. 3. Here we show the behaviors of energy, specific heat, entropy and chemical potential in Fig. 6. As can be seen in panel (a), the energy per particle E/NU increases monotonically with the temperatures. It is intuitive to notice that a larger hopping amplitude zJ/U leads to a lower energy. However, it is consistent with the behavior of entropy per particle S/Nk B shown in panel (c). The entropy increases as the temperature gets higher, with a larger hopping amplitude zJ/U corresponding to a smaller entropy. This is due to the fact that a larger hopping amplitude enhances superfluidity, leading to an ordered phase with a lower entropy. The specific heat per particle C V /Nk B shows a nonmonotonic behavior. It exhibits a peak at the transition temperature, indicating the disappearance of the superfluid order. At low temperatures, the chemical potential  www.nature.com/scientificreports www.nature.com/scientificreports/ increases sharply until it reaches a maximum at the transition, with a larger hopping amplitude corresponding to a lower chemical potential. At sufficient high temperature, the thermodynamics of the system is immune to the strength of hopping amplitude zJ/U.
Finally, we turn our focus to the thermodynamics for a supersolid phase. As shown in Fig. 7, the supersolid phase only exists in a limited regime of phase space, which is zJ/U ∈ (0.13, 0.20) in our case. Our numerical solution indicates that for zJ/U = 0.25 and zJ/U = 0.35, the system is in the conventional superfluid phase absent of the charge order. The energy per particle E/NU follows a monotonically increasing trend for all three typical values of zJ/U. The specific heat per particle C v /Nk B exhibits a characteristic cusp at the transition temperature at which the superfluid order parameter vanishes. The entropy per particle S/Nk B increases with temperature, indicating tendency toward disorder. The chemical potential manifests a nonmonotonic behavior with the maximum occurring at the transition temperature, and drops gradually with increasing temperature.

Summary
To sum up, we have studied the extended Bose-Hubbard model with global-range interactions at finite temperatures. We formulated a self-consistent mean-field theory to describe the finite-temperature physics. We have obtained temperature dependence of superfluid order parameters and number densities on even and odd lattice sites. Remarkably, we find that the melting of the charge order is gradually happened as the temperature is increased. For thermodynamic behaviors, we show the variations of energy, specific heat and entropy per particle Figure 5. (a) Energy per particle E/NU (b) specific heat per particle C V /Nk B (c) entropy per particle S/Nk B and (d) chemical potential as a function of varying temperatures for different global-range interaction strength K/U. At zero temperature, the system is in the phase of CDW (2,1) . The parameters used here are: zJ/U = 0 and the filling factor f = 1.5. Figure 6. (a) Energy per particle E/NU (b) specific heat per particle C V /Nk B (c) entropy per particle S/Nk B and (d) chemical potential as a function of varying temperatures for different hopping parameters zJ/U. At zero temperature, the system is in the superfluid state with Θ = 0. The parameters used here are: K/U = 0.2 and the filling factor f = 2.