Parity-time symmetry in a flat band system

Parity-time symmetry in a flat band system

Li Ge Department of Engineering Science and Physics, College of Staten Island, CUNY, Staten Island, New York 10314, USA The Graduate Center, CUNY, New York, New York 10016, USA
July 14, 2019

In this paper we introduce Parity-Time () symmetric perturbation to a one-dimensional Lieb lattice, which is otherwise -symmetric and has a flat band. In the flat band there are a multitude of degenerate dark states, and the degeneracy increases with the system size. We show that the degeneracy in the flat band is completely lifted due to the non-Hermitian perturbation in general, but it is partially maintained with the half-gain-half-loss perturbation and its “V” variant that we consider. With these perturbations, we show that both randomly positioned states and pinned states at the symmetry plane in the flat band can undergo thresholdless breaking. They are distinguished by their different rates of acquiring non-Hermicity as the -symmetric perturbation grows, which are insensitive to the system size. Using a degenerate perturbation theory, we derive analytically the rate for the pinned states, whose spatial profiles are also insensitive to the system size. Finally, we find that the presence of weak disorder has a strong effect on modes in the dispersive bands but not on those in the flat band. The latter respond in completely different ways to the growing -symmetric perturbation, depending on whether they are randomly positioned or pinned.

11.30.Er, 42.25.Bs, 42.82.Et

I Introduction

Systems that exhibit flat bands have attracted considerable interest in the past few years, including optical Manninen1 (); Manninen2 () and photonic lattices Rechtsman (); Vicencio (); Mukherjee (); Biondi (), graphene Kane (); Guinea (), superconductors Simon (); Kohler1 (); Kohler2 (); Imada (), fractional quantum Hall systems Tang (); Neupert (); Sarma () and exciton-polariton condensates Jacqmin (); Florent (). One interesting consequence of a flat band is the different scaling properties of its localization length when compared with a dispersive band Flach (); Leykam (); PRB15 (), due to a multitude of degenerate states in the flat band. This degeneracy has another important implication on Parity-Time () symmetry breaking Bender1 (); Bender2 (); Bender3 (); El-Ganainy_OL06 (); Moiseyev (); Kottos (); Musslimani_prl08 (); Makris_prl08 (); Longhi (); CPALaser (); conservation (); Robin (); RC (); Microwave (); Regensburger (); Kottos2 (); Peng (); Feng (); Hodaei (): it was found recently that the degeneracy of the underlying Hermitian spectrum, before any -breaking perturbations are introduced, determines whether thresholdless symmetry breaking is possible PRX14 (). Therefore, it is interesting to probe the interplay of the large degeneracy in a flat band system and symmetry breaking. In particular, we would like to know whether the degeneracy is completely lifted due to a -symmetric perturbation, and whether symmetry breaking depends on the evenness (oddness) of the degeneracy and its magnitude that grows with the system size. In addition, because a flat band makes the underlying Hermitian system more susceptible to disorder, it is equally important to understand the role of disorder on symmetry breaking in a flat band system.

Using a quasi-one-dimensional (quasi-1D) Lieb lattice (see Fig. 1) and a half-gain-half-loss perturbation (including its variant, the “V” configuration to be introduced below), we show in this paper that two different scenarios of thresholdless symmetry breaking can take place, depending on whether the degeneracy in the flat band is even or odd. When is odd, all but one flat band modes enter the -broken phase at the infinitesimal strength of the -symmetric perturbation. They form two degenerate branches, each confined strictly to either the gain half or the loss half of the lattice, and their non-Hermicity equals the strength of the -symmetric perturbation, which we denote by . The remaining flat band mode experiences an exceptional point of order 3 Graefe (), via the coupling with two dispersive band modes. When is even, all flat band modes experience thresholdless breaking, but now they exhibit four branches. Two branches are () degenerate and have the same properties as those in the -odd case. There is only one mode in each of the remaining two branches, and they form a -symmetric doublet, pinned at the symmetry plane () with exponential tails in both the gain and the loss halves. Surprisingly, we find that this localization is not due to the half-gain-half-loss nature of the -symmetric perturbation as previously found PRA11 (), but rather a result of the point defect at of this perturbation to satisfy the symmetry. Therefore, this spatial profile is insensitive to both and the system size when is large, and it can be reproduced in the underlying Hermitian system at . Using a degenerate perturbation theory, we derive this localization length and the rate these doublet states acquire non-Hermicity.

Finally, we show that the presence of weak disorder has a strong effect on modes in the dispersive bands but not on those in the flat band. The finite -transition thresholds of the former are smoothed out, while the thresholdless breaking of the latter is largely preserved. In addition, the flat band modes respond in completely different ways to increasing -symmetric perturbation when there is disorder. The -symmetric perturbation has little effect on them if they are already localized to either half of the lattice. Otherwise the perturbation forces them to pick a side, unless they are the doublet states, which evolve from Anderson localized states Anderson () to those pinned by the point defect at . We note that different from Refs. Makris_prl08 (); Szameit (); Zhen (), the system we consider here has a flat band before the -symmetric perturbation is introduced, instead of being the result of -symmetry breaking.

Figure 1: (Color online) Inset: A quasi-1D Lieb lattice with overlapping “” sublattices. Two dark states are shown schematically by circular clouds, which also serve as an example of a -symmetric “V” perturbation to be discussed in Section II. Main figure: Energy eigenvalues in a Lieb lattice with 10-fold degeneracy in the flat band. There is one more mode in each of the two dispersive bands. In all figures the energy is scaled by the coupling , where the onsite energies are all shifted to zero ().

Ii Thresholdless breaking in a Lieb lattice

In two-dimensional systems of a finite size, the maximum degeneracy due to a point group is 2. In a flat band, however, the degeneracy can be arbitrarily large, because it increases with the system size. Take a quasi-1D Lieb lattice for example (see Fig. 1), where an upright site is decorated to every other site of a 1D chain (i.e., the sites). A flat band exists when the onsite energy of and sites are the same, (), and gives the flat band energy. It is gapped from the two dispersive bands by , the real-valued coupling between two neighboring and sites. For simplicity we take as well. Because shifts all eigenvalues by the same amount and has no effect on the eigenstates, we take it to be zero. The degeneracy of the flat band in this Lieb lattice equals the number of existing dark states, which we will denote by due to their geometry (see the inset in Fig. 1). Each dark state has a nonvanishing amplitude only at a site and two nearest sites:


where the five elements are the amplitudes of the wave function on a “” sublattice, to which we will refer as an sublattice below. The sites are black in because the tunneling probabilities from the neighboring and sites cancel each other. The argument in is the position of the central site of an sublattice in the units of the lattice constant. It takes integer or half integer values, depending on whether is odd or even, and the center of the lattice is placed at . We note that the number of (overlapping) sublattices equals the number of dark states, and each end of the lattice is terminated on and sites. The superscript “” in Eq. (1) denotes the matrix transpose, and is the real-valued coupling between two neighboring and sites. Below we drop the vector symbol of without causing ambiguity.

The tight-binding Hamiltonian of the Lieb lattice can be written as


where runs through all unit cells, , and denotes Hermitian conjugate of the other terms in the square brackets. We then introduce the non-Hermitian perturbation , which is -symmetric about . is the overall strength of the perturbation, and is a diagonal matrix with positive (gain), negative (loss), and zero (no gain or loss) elements. To satisfy the -symmetry, no gain or loss is introduced on the lattice sites right at the symmetry plane at , which include one and one site when is even and a single site when is odd.

Figure 2: Thresholdless breaking in a Lieb lattice that completely lifts the degeneracy in the flat band with a general -symmetric configuration for (a) and (b) .

The degeneracy of the flat band modes is completely lifted by in general as they undergo thresholdless symmetry breaking, independent of whether is even or odd (see Fig. 2). The simplest -symmetric perturbation, with uniform gain on one half of the whole lattice and the same amount of loss on the other half, in fact partially maintains the degeneracy of the flat band. A variant of this half-gain-half-loss configuration with the same property is the “V” configuration (see Fig. 1; inset), which differs by having no gain or loss on all the sites (where the flat band modes are dark).

To see how the half-gain-half-loss configuration and the “V” configuration partially maintain the degeneracy of the flat band, we first note that a pair of modes are -symmetric partners, i.e., , because they are real-valued wave functions (see Eq. (1)). In addition, they are also eigenfunctions of for these two configurations, with opposite eigenvalues () when they do not overlap with the and site at . Therefore, they undergo thresholdless symmetry breaking simultaneously as increases from 0, and the imaginary parts of the corresponding energy eigenvalues are nothing but (see Fig. 3), independent of the system size and the couplings . In other words, their non-Hermiticy (given by ) is the same as the strength of the -symmetric perturbation (i.e., ). There are such pairs of flat band modes when is odd (e.g., 2 and 3 pairs for the cases shown in Figs. 3(a) and 6(a)) and such pairs when is even (e.g., 2 and 3 pairs for the cases shown in Fig. 3(b) and 6(b)), which all behave in the same way. As a result, each of the two branches has (-odd) or ( even) degeneracy in the -broken phase. Such a large number of degenerate states in the -broken phase has not been reported before.

Figure 3: (Color online) Thresholdless breaking in a Lieb lattice with the “V” configuration for (a) and (b) . (a) 4 flat band modes enter the -broken phase at (thick solid lines). The other flat band mode and all 12 dispersive band modes remain in the symmetric phase in the range of shown (thin solid line). (b) All 6 flat band modes enter the -broken phase at , 4 with (thick solid lines) and 2 with (dashed lines). All 14 dispersive band modes remain in the symmetric phase in the range of shown (thin solid line).

For the single dark state that is left alone in the -odd case, it is no longer an eigenstate of since there is no perturbation on the site at in order to respect the symmetry. Hence it needs to couple to modes in the dispersive bands to break the symmetry, which then leads to a finite threshold in terms of . In fact at this -symmetry breaking threshold lies an exceptional point of order 3 (EP) Graefe (), where the energy eigenvalues and wave functions of three modes coalesce, including two dispersive band modes and the solitary dark state (see Fig. 4). Nevertheless, a hybridized mode remains in the -symmetric phase after the EP, as if the solitary dark state remained in the -symmetric phase. We note that this EP does not occur if the onsite energy is detuned from and or with the half-gain-half-loss configuration.

Figure 4: (Color online) EP in a Lieb lattice with the “V” configuration and . The real and imaginary parts of the energy eigenvalues of two dispersive band modes and the solitary dark state are shown in (a) and (b) respectively, with the EP marked by the black dot. False color plots of the absolute value of their wave functions at (c) and (d) 1.58 are shown. The white sublattice in (c) indicates different lattice sites.

The two dark states and in the -even case are not eigenstates of either, due to the absence of perturbation on the site at in the “V” configuration (and the site at as well in the half-gain-half-loss configuration) in order to respect the symmetry. We will refer to these two states as the doublet states. Although they do not belong to the () degenerate manifolds of the two branches, they still experience a thresholdless breaking, but their is smaller than (see Fig. 3(b)). Interestingly, we find that the slope of these is also insensitive to the system size , when . More specifically, this slope is about when , measured by with the “V” configuration (see Fig. 3(b)), which is the configuration we will focus on below.

Figure 5: (Color online) Doublet states in the -broken phase with the “V” configuration. (a) False color plot of the absolute value of their wave functions for . The vertical dashed line marks , and the color scale is the same as in Figs. 4(c) and (d). (b) Same as (a) but for . (c) Exponential tails of the amplifying doublet state shown in (b) (solid lines). Only the absolute values of the wave function on the sites are shown. Circular dots and open triangles are calculated at and , respectively. The solid lines are proportional to shown for comparison. The dashed line shows the defect state at by increasing to 0.1.

To understand this property, we resort to two approaches, a qualitative one based on directly visualizing the spatial profiles of the doublets states, and a quantitative one based on a degenerate perturbation theory. As Fig. 5(a) shows, the doublet states are pinned near and have tails in both the gain and the loss halves of the lattice. We find that these spatial profiles are also insensitive to the system size when is large enough (; see Figs. 5(a) and (b)), which explains the same property of their . In fact, we find the tails of their spatial profiles decay exponentially away from (see Fig. 5(c)). One might expect that these exponential tails are a result of gain and loss, as it has been shown that the wave function in the -broken phase tends to peak at the gain and loss interface PRA11 (). However, we find that the exponential tails are largely independent of the -symmetric perturbation strength, either. As Fig. 5(c) shows, the tails are captured well by an exponent of , and there is little change in the wave function when changes from to . Instead, we find that this localization length of is due to the point defect of the “V” configuration at , which has neither gain or loss on the site at in order to respect the symmetry as mentioned. If we introduce a point defect at in the Hermitian system at , for example, by increasing here to 0.1, we recover the same localization length (see the dashed line in Fig. 5(c)).

Before we derive the perturbation theory for the doublet states, we briefly discuss the modes in the dispersive bands. They have high -transition thresholds when is small. This observation can be understood in the following way: their eigenvalues are distributed in (see Fig. 1) and are well separated from each other when is small; their thresholds are proportional to these spacings, in the simplest case of two-mode coupling PRX14 (). As increases, their energy spacings reduce and so do their -transition thresholds. For example, no dispersive band modes enter the -broken phase in Fig. 3, but their lowest threshold reduces to and for and , respectively (see Fig. 6). Due to the symmetry of the dispersive bands about (see Fig. 1), when one pair of dispersive band modes enter the -broken phase at some finite value of , there is always another pair that do the same at exactly the same but on the opposite side of the flat band energy ; their are nevertheless the same. Different from the EP scenario depicted in Fig. 4 in which two dispersive band modes are also involved, here the real parts of their energy eigenvalues are different from in the -broken phase (not shown).

Figure 6: (Color online) Same as Fig. 3 but with (a) and (b) . (a) 4 and (b) 8 dispersive band modes enter the -broken phase before (dash-dotted lines). Note that the features of the flat band modes (solid and dashed lines) are the same as in Fig. 3. The horizontal thin lines represent modes in the -symmetric phase.

Iii Degenerate perturbation theory

Now we turn to the perturbation theory for a more quantitative understanding of the doublet states, and hence the considered in this section is even. We start by diagonalizing the perturbation in the -fold flat band subspace of , which is required in the degenerate perturbation theory Shanker (). In the case, we define the basis in this subspace as and , where we can take to be real numbers, because (without the factor ) is Hermitian. The superscript enclosed in parentheses indicates the value of . The above requirement then means , and an additional constraint is . We note that this requirement is different from demanding that are the eigenstates of ; the latter is sufficient but unnecessary.

Since the flat band states are dark on sites, we can project the wave functions and to the Hilbert space of and sites, leading to , , and when , where “diag” stands for a diagonal matrix. Using we find , and leads to


Note that the two values of are reciprocal to each other, which means that if one leads to , the other one gives . By neglecting the coupling to the dispersive band modes, we then derive


for the doublet states, which gives a slope of when . Using in the expression above leads to the same result. Previously we have mentioned that the numerically obtained slope in this case is , calculated using . If we reduce the perturbation strength at which the slope is calculated, for example, to , we find , which agrees nicely with the analytical result given by Eq. (4). Since the slope of given by Eq. (4) is independent of , we know that any change to the slope must be a result of coupling to the dispersive bands, which is neglected in the derivation of Eq. (4). Nevertheless, the small difference between at and 0.1 indicates that such coupling is weak.

For , the construction of the first basis functions in the -fold flat band subspace is straightforward: any dark states that do not overlap with are eigenfunctions of , as we have mentioned. These dark states just need to be linearly superposed properly such that they form orthogonal basis functions, and there is more than one way to achieve it. For the remaining two doublet states, we use mathematical induction to find their approximate forms. Assuming that we have solved the case and found the correct doublet states , we then approximate the correct doublet states in the case by


where are two real numbers. The basic assumption is that the central part of near is insensitive to , as we have seen in Figs. 5(a) and (b). It is easy to check that , using , and by requiring , we find


where are the first (last) and last (first) elements of (). An additional constraint imposed by the degenerate perturbation theory is that need to be orthogonal to the first basis functions in the -fold flat band subspace. Let us pick, for example, one such basis function simply as (which is an eigenfunction of ), and we immediately find from and from when . We note that we arrive at the values of and with other choices of , such as or . Once and are found, we can immediately construct the leftmost and rightmost elements of and to derive the localization length for the doublet states. For example, the first four elements of are . The localization length can then be defined as


using the values of the wave function on the first site (i.e., ) and the second site (i.e., ) from the left. Equation  (8) gives , which agrees reasonably well with the result of numerical fitting of the exponential tails shown in Fig. 5(c), i.e., . In the Appendix we give another way to estimate this localization length.

For the slope of the doublet states, a recursive relation can then be formulated. Assuming is amplifying, we find


It is clear that (and similarly ) becomes insensitive to as becomes large, because are at the very ends of the exponentially decaying tails of , i.e., , leading to a converging series . Using given by Eq. (4), we successively find , , , which agree well with the previously mentioned numerical values.

Iv Effect of disorder

Figure 7: (Color online) (a)–(c) Evolution of the dark states in the degenerate flat band manifolds from , 0.01, to 0.075. Two typical examples are shown. (d)–(f) Same as in (a)–(c) for the doublet states. The color scale and legend are the same as in Figs. 5(a) and (b). The amplitude of onsite white noise is and .

Unlike the doublet states, the -broken dark states in the two degenerate manifolds can be randomly positioned along the lattice, but they are strictly confined on either the gain or the loss half of the lattice. Due to their degeneracy, any arbitrary superpositions of them are still eigenstates of the system, and one can always find pairs of them such that they are -symmetric partners of each other. However, the relevant superpositions are determined by the disorder in the system. Here we consider weak disorders by including a white noise with a uniform distribution in around on each lattice site. As the lower mode in Figs. 7 (a)–(c) shows, if a flat band mode in the two degenerate manifolds is already confined to the loss (or gain) half of the lattice at small , increasing has little effect on its spatial profile. However, if at small one of these modes occurs in both the gain and loss regions, it will be forced to take either the gain half or the loss half, as the upper mode in Figs. 7 (a)–(c) shows. Here the prevailing effect of is its non-Hermicity, separating the lattice into a gain half and loss half.

In contrast, the prevailing effect of on the doublet states is its point defect mentioned previously. At very small , the doublet states are localized by disorder, i.e., they are Anderson localized Anderson (), and the localization length can be rather long in a particular disorder realization (although on average the localization length is not much longer than that determined by the point defect PRB15 ()). As increases, the point defect in gradually prevails over the white noise disorder, and the doublet states approach their spatial patterns in the absence of , as can be seen from Figs. 7(e) and 7(f) in comparison with Fig. 5. In other words, the -symmetric relation of the doublet states is restored as increases. The same cannot be said about the other flat band modes in general, due to the presence of disorder that breaks the symmetry.

Figure 8: (Color online) Same as Fig. 6 but with disorder. The amplitude of onsite white noise is .

Finally, we find that weak disorder has a stronger effect on the dispersive bands than the flat band in terms of breaking. As Fig. 8 shows, the disorder smoothes out the -transitions of the dispersive band modes in Fig. 6, but the thresholdless breaking of the flat band modes is largely unaffected. These contrasting behaviors are due to the different routes to -symmetry breaking, i.e., whether an exceptional point is involved. On the one hand, an exceptional point is very sensitive to perturbations, and it quickly becomes an avoided crossing in the complex eigenvalue plane when the -symmetry of the system is lifted by the weak disorder. In fact, each bifurcation of we have seen in Fig. 6 from a finite is for two pairs of dispersive band modes as mentioned at the end of Section II. Now in the presence of weak disorder, the sensitivity of the exceptional points breaks each of these bifurcations into two, and we see four and eight trajectories of in Figs. 8(a) and (b) (dash-dotted lines) instead of two and four in Figs. 6(a) and (b). On the other hand, the thresholdless -symmetry breaking of the flat band modes does not involve an exceptional point; its role is replaced by the Hermitian degeneracy at PRX14 (). In this case there is no singularity, and we have seen that the first-order perturbation theory describes the thresholdless -breaking well in Section III. Now with the weak disorder, its leading (i.e., linear) effect is merely perturbing the real part of the energy eigenvalues, similar to how the -perturbation varies the imaginary part of the energy eigenvalues. Therefore, these two perturbations are independent processes to the leading order, and the thresholdless -breaking is largely unchanged with the weak disorder. As the strength of -breaking increases with , the effect of the weak disorder is further suppressed. This can be seen from the following observation. We find that one flat band mode with in Fig. 8(b) deviates slightly from the other 2 in this branch at small but rejoins the latter as increases. This behavior is due to its spatial profile change caused by the increasing perturbation, similar to that of the upper mode in Figs. 7(a)–(c): when this mode has a small portion in the gain half of the lattice at small , overall it experiences less loss and hence its negative is larger than . As its spatial profile is squeezed into the loss half of the lattice by the growing -symmetric perturbation, it experiences more loss than before and its approaches its minimum value . We can also infer that the other 2 modes in this branch are localized already in the loss half when is small, which is verified by inspecting their spatial profiles (not shown).

V Conclusion

We have mentioned that the degeneracy of the flat band modes is completely lifted by a -symmetric perturbation in general as they undergo thresholdless symmetry breaking. An exception takes place in the half-gain-half-loss configuration and its “V” variant, where two different scenarios of thresholdless symmetry breaking occur in the flat band, depending on whether the degeneracy in the flat band is even or odd. The two degenerate manifolds with always exist and undergo thresholdless breaking. While their center positions are random, they are confined to either the gain half or the loss half of the lattice in the absence of disorder. This feature holds even with weak disorders, when the -symmetric perturbation is strong enough. In contrast, the -symmetric doublet states only exist when is even, and they display weaker non-Hermicity than the degenerate manifolds. These doublet states are pinned at the symmetry plane with exponential tails in the gain and the loss halves. These tails are the result of a point defect in the -symmetric perturbation at , instead of its half-gain-half-loss nature as previously found PRA11 (). Weak disorders may disturb their spatial profiles at small -symmetric perturbation, but as the latter increases, this feature is restored, together with the -symmetry relation between the two doublet states.

The author thank Hakan Türeci, Bo Zhen, and Vadim Oganesyan for helpful discussions. This project is partially supported by NSF under Grant No. DMR-1506987 and by the Collaborative Incentive Research Grant of City University of New York, CIRG-802091621.

Appendix: Localization length of the defect states

In the main text we estimated the localization length of the doublet states by a degenerate perturbation theory. This localization length can also be estimated, for example, using the iterative relation for the values of the wave function on sites. To derive this iterative relation, we apply the effective Hamiltonian to all the lattice sites:


where represents any perturbation to the diagonal elements of (including the “V” configuration and the Hermitian defect discussed in Fig. 5) and is the wave function on the th site of type . , where is an eigenvalue of and is the onsite energy of . can have an imaginary part to represent gain or loss if present.

By solving the Eqs. (10) and (11), we find


By substituting and in Eq. (12) with this expression, we find the recursive relation for the values of the wave function on sites:


For the doublet states and its Hermitian counterpart shown in Fig. 5, since it is the same for all lattices on the left (right) side of , and . We can then rewrite Eq. (14) as


Defining the localization length as for and assuming , we find


using Eq. (16), and it gives when . This result holds whenever there is a defect state in the Lieb lattice, and it applies to the point defect in both of the “V” configuration and the Hermitian defect we discussed in Fig. 5. The difference of these two cases lies in the values of , which are not important for as long as . Finally, we note that by defining a complex wave vector for , Eq. (17) can be interpreted as solving the band structure of the dispersive bands inversely band (): instead of finding the energy of a band at a given wave vector, one can find the wave vector at a given energy; if this energy is in the band gap, one finds that has to be purely imaginary and its absolute value is given by Eq. (17) when .


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