Short-time dynamics in s+is-wave superconductor with incipient bands

# Short-time dynamics in $s+is$-wave superconductor with incipient bands

## Abstract

Motivated by the recent observation of the time-reversal symmetry broken state in K-doped BaFeAs superconducting alloys, we theoretically study the collective modes and the short time dynamics of the superconducting state with -wave order parameter using an effective four-band model with two hole and two electron pockets. The superconducting state emerges for incipient electron bands as a result of hole doping and appears as an intermediate state between (high number of holes) and (low number of holes). The amplitude and phase modes are coupled giving rise to a variety of collective modes. In the state, we find the Higgs mode at frequencies similar to a two-band model with an absent Leggett mode, while in the and state, we uncover a new coupled collective soft mode. Finally we compare our results with the solution and find similar behaviour of the collective modes.

###### pacs:
05.30.Fk, 32.80.-t, 74.25.Gz

## I Introduction

Ultrafast pump-probe experiments recently become a powerful tool to probe the temporal dynamics of symmetry broken states and relaxation in conventional and unconventional superconductorsPashkin et al. (2010); Beck et al. (2011); Fausti et al. (2011); Matsunaga and Shimano (2012); Dal Conte et al. (2012); Beck et al. (2013); Matsunaga et al. (2013); Mansart et al. (2013); Matsunaga et al. (2014); Hu et al. (2014); Casandruc et al. (2015); Matsunaga et al. (2017). For high frequency excitation with frequency exceeding the superconducting gap, , the radiation breaks Cooper pairs into quasiparticles, which yields rapid dissipation and thermalization of the system. However, an intense pulse as used in Ref.Matsunaga et al. (2013) couples non-linearly to the Cooper pairs of the superconductor. This, as was argued theoretically, should lead to a coherent excitation of the Higgs amplitude mode Volkov and Kogan (1974); Amin et al. (2004); Barankov et al. (2004); Yuzbashyan et al. (2005, 2006); Barankov and Levitov (2006); Papenkort et al. (2007); Krull et al. (2014); Yuzbashyan et al. (2015); Tsuji and Aoki (2015a); Murotani et al. (2017); Chou et al. (2017). In the experiments Matsunaga and Shimano (2012); Matsunaga et al. (2013, 2017) the detection is performed over a window of about 10 picoseconds (ps), well before thermalization occurs (likely due to acoustic phonons on a timescale of 100 psDemsar et al. (2003)).

While non-equilibrium collective modes in conventional single-gap superconductors are relatively well understood, the investigation of collective excitations in unconventional non-equilibrium superconductors with multicomponent or multiple gaps is a very intriguing topic due to a very rich spectrum of the collective excitations Akbari et al. (2013); Dzero et al. (2015); Demsar (2003); Leggett (1966); Anishchanka et al. (2007); Krull et al. (2017). Fe-based superconductors are particularly interesting in this regard due to its variety and complexity of their phase diagrams. For example, recent experimental studies of the Fe-based superconductors have demonstrated the emergence of superconducting state with incipient bands, i.e. bands which do not cross Fermi level. Okazaki et al. (2014); Miao et al. (2015) Furthermore, the formation of the incipient bands is often connected to the Lifshitz transition, where one of the bands continuously moves away from the Fermi level as a function of doping Lifshitz (1960). A peculiar example of an iron-based superconductor with a Lifshitz transition is BaKFeAs where the Fermi surface topology changes from the one having both the electron and the hole pockets to the one where the electron pockets sink below the Fermi level. Angle-resolved photoemission (ARPES)Sato et al. (2009); Xu et al. (2013) and thermopowerHodovanets et al. (2014) measurements point toward the existence of such a transition in the overdoped hole-doped compounds with . Intriguingly, in the same doping range, the structure of the superconducting gaps undergoes dramatic changes, seemingly inconsistent with a two-band description. While multiple experiments supports the nodeless -wave superconducting gap near the optimal doping Nakayama et al. (2011); Ding et al. (2008); Christianson et al. (2008); Luo et al. (2009), the situation is very different for the extremely overdoped case. In this doping range the experiments indicate either strongly anisotropic wave Cooper-pairing with sign change on the remaining two hole pocketsOkazaki et al. (2012); Watanabe et al. (2014); Cho et al. (2016) or the -wave pairing with well-defined nodesReid et al. (2012); Tafti et al. (2013) on the hole Fermi surface sheets. Moreover, in the intermediate doping region, frustration between the two superconducting channels has been theoretically predicted to result in a time-reversal symmetry-breaking stateStanev and Tesanovic (2010); Carlström et al. (2010); Hu and Wang (2012); Maiti and Chubukov (2013); Böker et al. (2017) or statePlatt et al. (2009); Thomale et al. (2011). In these states, the phase difference between the order parameters at the two hole bands is not equal to a multiple of with the symmetry being spontaneously broken.

The time-reversal symmetry breaking and states possess several interesting properties and should demonstrate an unusual dynamics. For example, as a result of simultaneous breaking of and symmetries, the vortex fractionalization and unusual vortex cluster states have been predicted to exist for the stateCarlström et al. (2010). The collective excitations of the phase differences between order parameters of different bands (Leggett modes) in the state is expected to have peculiar phase-density natureCarlström et al. (2010) and have been predicted to soften at the critical pointsMaiti and Chubukov (2013); Böker et al. (2017). The time-reversal symmetry breaking is most directly manifested in spontaneous currents around nonmagnetic impuritiesMaiti et al. (2015) or quench-induced domain wallsGaraud and Babaev (2014). The currents result in local magnetic fields in the superconducting phase and provide a signature of the time-reversal symmetry broken state. Recent results in BaKFeAs are consistent with state or state at x = 0.73Grinenko et al. (2017), close to the region where the Lifshitz transition is considered to occur. This observation stimulates to analyze further details of the time-reversal symmetry broken states in strongly overdoped iron-based superconductors.

Given these theoretical and experimental developments, in this paper we study the signatures of the Cooper-pairing in the pump-probe spectroscopy. Specifically, we adopt the four-band model developed in Ref. Böker et al., 2017 to analyze the pairing dynamics. In addition, we also analyze the nature of the collective excitations. One of the our main findings are the emergence of the pairing when initially the superconductor is in the state and existence of the sharp collective in the state. In addition, we also studied the pump-probe dynamics in the state and find that this state shows a very similar soft mode dynamics as it is the case for the state.

Our paper is organized as follows. Sections II and III contain a description of the model and its ground state within the mean-field theory approximation. In Section IV we study the non-adiabatic dynamics of the of a superconductor initiated by a sudden change of the pairing strength or an application of an external electromagnetic field. In Section V we present our results for the collective excitations depending on the doping level. Section VI is devoted to the discussion of our results.

## Ii Model

We consider a model of a metal with four bands - two hole-like and two-electron like - with fully local particle-particle interactions. The model Hamiltonian is: Böker et al. (2017)

 ^H=∑k,a,σξak^ca†kσ^cakσ++∑kk′∑ab(Uab^ca†k↑^ca†−k↓^cb−k′↓^cbk′↑+h.c.). (1)

Here are the band labels, () are the fermionic creation (annihilation) operators, are coupling constants and are the single particle dispersions in each band. In what follows, we simplify our model by considering two identical electron- and hole-like bands within the tight-binding approximation:

 ξhik=th(2−coskx−cosky)+ED2−μ,ξeik=te(2−coskx−cosky)−ED2−μ, (2)

where , are the hopping amplitudes, is the chemical potential and accounts for the changes in the relative occupation numbers of the electron and hole bands.

Lastly, we set the coupling constants as

 Uh1h1=Uh2h2=0,Ue1e1=Ue2e2=0,Uh1h2=Uh2h1=Uhh,Ueihj=Uhjei=Ueh (3)

(in the last expression ). Having formulated the model, we now review its ground state properties within the mean-field approximation.

## Iii Mean-field theory

Using the standard methodology, we decouple the two-fermion interaction term (1) in the particle-particle channel introducing the following mean-field pairing amplitudes: and (). Minimizing the free energy with respect to the mean-field amplitudes yields the following system of equations

 Δe=−Ueh(Δh1Ih1+Δh2Ih2),Δh1=−2UehΔeIe−UhhΔh2Ih2,Δh2=−2UehΔeIe−UhhΔh1Ih1. (4)

where we introduced

 Ia=∑ktanh(Eak/2kBT)2Eak,a∈{e,h1,h2} (5)

for brevity and are the single-particle energies. The mean-field equations (4) have to be supplemented by the particle-number equation which determines the changes in the chemical potential due to the onset of superconducting order. It turns out to be convenient to evaluate the chemical potential as a function of the carrier number (per spin), i.e. the difference between the electrons and holes:

 nc=∑k[ξekEektanh(Eek2kBT)++ξhk2Eh1ktanh⎛⎝Eh1k2kBT⎞⎠+ξhk2Eh2ktanh⎛⎝Eh2k2kBT⎞⎠⎤⎦.

The detailed analysis of mean-field equations (4) can be easily performed numerically. Upon closer inspection of these equations, however, it becomes clear that one can basically guess the solution of these equations without resorting to numerics. Indeed, for the values of the chemical potential well below the bottom of the electronic bands, it is clear that there should be no pairing on the electronic pockets, , so from the mean field equations it follows that , while the will be given by the root of . Thus, for the superconductivity is described by order parameter. Let us now consider the opposite limit of filled electronic band, . Without any loss of generality, let us consider the pairing order parameter on the electron pockets to be purely real. Furthermore, the structure of the mean-field equations suggests that the pairing amplitudes in the hole bands must be the same:

 Δe=|Δe|,Δh1=|Δh|eiϕ1,Δh2=|Δh|eiϕ2. (6)

We can now insert these equations into (4) and separate the real and imaginary parts. It then follows that for the phases the following relation must hold

 ϕ1=−ϕ2=φ/2, (7)

where the relative phase is determined by

 cos(φ2)=−Uhh2Ueh⋅|Δe||Δh|, (8)

while the amplitudes and are the roots of the following two equations: and

 |Δe|⋅[1−2U2ehIe(Δe)Ih(Δh)]=0. (9)

Clearly, these equations have a root corresponding to the state and a conventional -wave state . It is therefore natural to expect that there also should be a solution corresponding to the intermediate values of phase . By analyzing the mean-field equations above numerically, we have confirmed that it is indeed the case and, moreover, the solution corresponding to the state with has the lowest energy. In Fig. 1 we present the results of the numerical analysis of the mean-field equations.

Having reviewed the mean-field results for the model, we turn our discussion to the analysis of the collective response of the superconductor.

## Iv Temporal evolution of the s+is order parameter

In this Section we discuss the short-time dynamics of the superconductor initiated by either sudden change of the pairing strength or by a short pulse of an external electromagnetic field. Although at first glance these two ways of driving a system out-of-equilibrium seem to be very different, one can employ the linear analysis of the equations of motion, i.e. consider the limit of weak deviations from the ground state, to demonstrate that for the time-dependent correction to the ground state pairing amplitude external pulse has is many ways the same effect as a quench of the pairing strength. Tsuji and Aoki (2015b)

To study the short time dynamics of a superconductor within the mean-field approximation described above, it is convenient to use the Anderson pseudospin variables. Anderson (1958) In terms of these variables, the equations of motion are

 ∂tSlk=Blk×Slk, (10)

where and . The - and -component of are given by the mean-field self-consistency equations

 Δ±h1(t)=∑k[−2UehS±ke(t)−UhhS±kh2(t)],Δ±h2(t)=∑k[−2UehS±ke(t)−UhhS±kh1(t)],Δ±e(t)=−Ueh∑k[S±kh1(t)+S±kh2(t)] (11)

and we use the shorthand notation . In the equilibrium a given pseudospin is collinear with the corresponding , so the sudden change of one of the coupling constants entering into (11) brings a system far from its equilibrium state.Barankov et al. (2004); Yuzbashyan et al. (2015)

Given that the region in the parameter space of the relative band occupation numbers where the pairing state is a ground state is quite narrow, we asked ourselves whether pairing amplitude will emerge dynamically when initially a superconductor is in the pairing ground state. To address this question, we solved the equations of motion numerically on a discreet mesh of momentum points. The results of the calculation are shown in Fig. 2. We indeed observe the dynamical onset of the -pairing state, albeit this onset happens rather slowly. Specifically, it emerges on a time scale which far exceeds where is an equilibrium value corresponding to a ground state with the new coupling .

In order to verify this result, we have performed the stability analysis by considering the pseudospin configuration corresponding to the state and allowing for small fluctuations into the state. Since numerical calculations show that increases exponentially with time, we assume that

 δΔ±e(t)=d±ee(γ±iω)t,de≪|Δh| (12)

and both and are some real parameters which we need to determine. Employing the equations of motion, it is easy to show that the linear correction to the pseudospins on the electronic bands are

 δS±ke(t)=±δΔ±e(t)iγ∓ω±2ξek. (13)

Similarly to (13), the correction to the pseudospins on the hole bands are found to be

 δS±kh1(t)=∓2δΔ±h1(t)Shkziγ∓ω±2ξhk,δS±kh2(t)=∓2δΔ±h2(t)Shkziγ∓ω±2ξhk. (14)

By inserting these expressions into the self-consistency equations (11), one arrives at the system of linear equations for the linear corrections to the pairing fields on each pocket. These equations will have non-trivial solution provided the determinant of the corresponding matrix is zero. This condition has the form of the following equation

 [1−Uhhχh(ζ)][1+Uhhχh(ζ)−4U2ehχe(ζ)χh(ζ)]=0, (15)

where , and . The reader can easily check that this equation does not have a solution for which means that the remains perfectly stable. However, for such that the superconducting state is a ground state, we found that (15) has a root and .

## V Collective modes

### v.1 Response to fast perturbations: non-adiabatic regime

We now turn our discussion to the question of the collective response of the superconductor. Therefore, we perturb the system with a pump pulse to simulate the THz experiment. The electric field of this laser pulse can be described by a time dependent vector potential . We choose the spectrum of this pulse to be a Gaussian envelope centered around a frequency close to ,

 A(t)=A0θ(−t)e−(t−t0)22τ2cos(ω0t). (16)

Here, controls the width of the time dependent signal and therefore needs to be chosen in such a way, that the signal disturbs the system non adiabatically. Also, we choose small enough to not change the ground state, i.e., . The electromagnetic vector potential couples to the system via minimal substitution, i.e., . This changes the pseudo magnetic field in the equations of motion (10) into

 Blk=(−2Δlx,−2Δly,(ξk+ecA(t)l+ξk−ecA(t)l)). (17)

The numerical solution of the non-equilibrium dynamics are shown in Fig. 3. One clearly see that both the dynamics of the amplitude and the relative phase are dominated by one frequency . All oscillations are undamped, because the frequency is smaller than , i.e., the smallest possible Higgs-mode and the beginning of the quasiparticle continuum. However, the absence of damping is a peculiarity of the model, since we assume isotropic -wave order parameters. In the real system the nodal character of the order parameters leads to dampening effects.

We examine the mode by numerically solving the equations of motions over the whole phase. The result is shown in Fig. 4. Obviously, the mode softens close to the borders of the -state and has its maximum value deep inside the -regime. The coupling of both - amplitude and relative phase oscillations - is a peculiarity of the collective excitations in time reversal symmetry broken systems and differs from the usual dynamics of multiband superconductors. Also the softening of the mode close to the borders of the state can be explained by the second order phase transition from the into the state Carlström et al. (2010); Maiti and Chubukov (2013); Böker et al. (2017). For comparison we shown in Appendix In B that this result still holds if the system, via an intermediate s+d-state, ends up in a d-wave symmetry at large hole doping.

### v.2 Collective response in the adiabatic regime

To study to collective mode at long wavelength limit, we linearize equations of motion (10 ) with respect to the deviations from the equilibrium, , , and the effect of perturbation potential, . The deviations are homogeneous in space so they describe the collective mode at long wavelength limit. The details of the calculations can be found in the Appendix A. Here we discuss our main results.

The resulting linearized equations will have non-trivial solution provided the corresponding determinant vanishes which sets us the non-linear equation for the frequency of the collective modes. We solve the equation for mode, Eq. (21), for all the ground states pseudospin configurations - , and - and near the transitions between these states. In all three states, we find a solution at : this mode is an overall phase mode without changing amplitude and relative phase difference, so this motion does not cost any energy. It is the Goldstone mode from U(1) symmetry breaking of BCS ground state. Beside this, we also find a new low energy mode as shown in Fig. 5. The energy of this mode decreases at the boundary of state.

In state, we find that the mode is the motion of antisymmetric phase change of two hole bands gaps coupled with amplitude change of electron band gap. We have the eigenvector of mode, , where , are positive real values, see Fig. 6. Similarly, in state, we find the mode is the motion of antisymmetric phase change of two hole bands gaps. We have the eigenvector of mode

In state, the mode is an amplitude-phase coupled mode between both incipient electron and partially filled hole bands. Therefore it corresponds to in Section V.1. The eigenvector is

 δ→Δs+is=[δΔxe,δΔyeeiπ2,δΔxheiϕ,δΔyheiϕ,δΔxhe−iϕ,−δΔyhe−iϕ]. (18)

Note that the first two components of has a relative phase of which is a direct consequence of the incipiency of the electron band, as follows directly from the structure of the matrix elements (21) and the fact that in that matrix is purely imaginary. Unlike the overall phase mode, this low energy mode vector is not continuous at the boundary between the two states. Near the boundary of and state, , the mode is a combination of mode and overall phase mode, see Fig. 7. At the end, it is not surprising because of both overall phase mode and low energy mode are soft at the boundary. As increasing, , decrease and , increase. Near the boundary of and state, , the mode is a combination of mode and overall phase mode, Fig. 7.

## Vi Discussion and Conclusion

It is well known, the problem of non-adiabatic dynamics of the BCS model is exactly solvable Yuzbashyan et al. (2006). The model presented above can be also shown to be exactly integrable for a special choice of the coupling constants, which however, do not describe the regime where state has the lowest energy. Nevertheless, we have checked that despite the lack of the integrability in our model, the non-equilibrium dynamics of the order parameter, which is initiated by a sudden change of the pairing strength bears a lot of similarities with the results obtained from exactly solvable version of the model.

Another important aspect related to similarities and differences for the short-time order parameter dynamics between integrable and non-integrable models is concerned with the emergence of the state in the incipient electronic band. Indeed, within the both single-channel and two-channel pairing models for the degenerate atomic Fermi gases Yuzbashyan et al. (2015) the realization of the steady state with periodically oscillating amplitude is limited to the weak-to-moderately strong coupling quenches in the vicinity of the BCS-BEC crossover. Our results show that, on one hand we have a steady state with periodically oscillating pairing amplitude, while on the other hand, the electronic band is incipient mimicking the BEC limit in atomic gases. Thus observation of this effect may question the interpretation of the state as being analogous to the BEC pairing in atomic condensates.

It is also important to keep in mind that the observation of the collective oscillations during the pump-probe experiments can in principle be inhibited by two effects: (i) spatial inhomogeneities of the pairing amplitude which may develop by parametric instabilities Dzero et al. (2008) and (ii) the Coulomb interactions between the particles. The effects of the Coulomb interactions on the non-equilibrium dynamics still remains a largely open problem. However, since our model involves purely repulsive interparticle interactions, we believe that the effects of the Coulomb interactions will not affect the dynamics in a profound way.

To conclude, we theoretically study the collective modes and the short time dynamics of the superconducting state with -wave order parameter using an effective four-band model with two hole and two electron pockets motivated by the recent experiments on time-reversal symmetry broken state in iron-based superconductors. The superconducting state emerges for incipient electron bands as a result of hole doping and appears as an intermediate state between (high number of holes) and (low number of holes). The amplitude and phase modes are coupled giving rise to a variety of collective modes. In the state, we find the Higgs mode at frequencies similar to a two-band model with an absent Leggett mode, while in the and state, we uncover a new coupled collective soft mode. We also compare our results with the solution and find similar behavior of the collective modes.

Acknowledgments. We are thankful to I. Paul and T. Tohyama for discussions. The work of P. S. and M. D. has been financially supported by the National Science Foundation grant NSF DMR-1506547. The work of M.D. was financially supported in part by the U.S. Department of Energy, Office of Science, Office of Basic Energy Sciences under Award No. DE-SC0016481. M.A.M. and I.E. were supported by the joint DFG-ANR Project (ER 463/8-1) and DAAD PPP USA N57316180.

## Appendix A collective mode in continuous model at q=0

The linearized equations of motion are

 ∂tδSxkl(t)=−2ΔylδSzkl(t)−2SzklδΔyl(t)−2ξklδSykl(t)−2SyklδBzkl(t),∂tδSykl(t)=2ξklδSxkl(t)+2SxklδBzkl(t)+2ΔxlδSzkl(t)+2SzklδΔxl(t),∂tδSzkl(t)=−2ΔxlδSykl(t)−2SyklδΔxl(t)+2SxklδΔyl(t)+2ΔylδSxkl(t) (19)

Fourier transformation, e.g., , give

 ⎛⎜ ⎜⎝δSxkl(ω)δSykl(ω)δSzkl(ω)⎞⎟ ⎟⎠=Szklξkl(4E2kl−ω2)⎛⎜ ⎜ ⎜⎝4(ξ2kl+Δyl2)2iωξkl−4ΔxlΔyl2iωΔyl+4Δxlξkl−2iωξkl−4ΔxlΔyl4(ξ2kl+Δxl2)−2iωΔxl+4Δylξkl−2iωΔyl+4Δxlξkl2iωΔxl+4Δylξkl4(Δxl2+4Δyl2)⎞⎟ ⎟ ⎟⎠⎛⎜ ⎜⎝−δΔxl(ω)−δΔyl(ω)δBzkl(ω)⎞⎟ ⎟⎠ (20)

We take since the collective mode should not depend on the perturbation and substitute the result into self-consistency equation (11 ), we obtain

 (21)

where the quantities in the equation at T=0 are given by

 Mαl(ω)=∑k2[ξ2kl+(Δαl)2](4E2kl−ω2)Ekl,Γl(ω)=∑kiωξkl−2ΔxlΔyl(4E2kl−ω2)Ekl (22)

and .

In usual one band or two bands superconductor, after choosing proper gauge, due to electron-hole symmetry, thus the amplitude and phase are decoupled in the equation. In the time reversal symmetry broken system, one can not choose a gauge to vanish all . Besides, the broken electron-hole symmetry of the incipient electron band makes always non-vanishing. As a result, the amplitude and phase oscillation are coupled in the mode. The frequency of the mode is determined by the solution of equation

 Det[M]=0 (23)

where is the 66 matrix in (21). The eigenvectors of the matrix

 δ→Δ(ω)=[δΔxe(ω),δΔye(ω),δΔxh1(ω),δΔyh1(ω),δΔxh2(ω),δΔyh2(ω)] (24)

tell how amplitude and phase are coupled in the collective excitation.

## Appendix B collective modes inside the s+id regime

In this section we discuss the collective dynamics inside a s+d superconductor. Therefore, we modify the Hamiltonian (1) and add another channel to the inter-hole-band interaction to allow for d-wave pairing

 Uh1h2k,k′ ≡Uhh,s+Uhh,dcos(2ϕk)cos(2ϕk′), (25)

where are constant and . This leads to momentum dependent order parameters for the two hole bands

 Δhik=Δshi+iΔdhicos(2ϕk), (26)

where and are the s- and d-wave pairing amplitude. It is important that the only possible pairing symmetry with mixed s- and d-wave component is s+d, since s+d symmetry breaks the -symmetry of the system. Also we choose the d-wave component large enough to suppress a possible competition between s+s and s+d superconductivity, i.e., we can choose and real. This argument can also be shown by free energy analysis. The pairing amplitude for the electron-band remains constant and is chosen positive to fix the overall phase.
Minimizing the free energy with respect to the five different pairing amplitudes we obtain

 Δe =−Ueh(Δsh1Ih1+Δsh2Ih2), Δsh1 =−2UehΔeIe−Uhh,sΔsh2Ih2, Δsh2 =−2UehΔeIe−Uhh,sΔsh1Ih1, (27) Δdh1 =−Uhh,dΔdh2Jh2, Δdh2 =−Uhh,dΔdh1Jh1,

where was introduced in Eq. (5) and

 Ja=∑ktanh(Eak/2kBT)2Eakcos2(2ϕk). (28)

Since the order parameters are momentum dependent, the single-particle energies of the hole-bands now have the form .
Again, we take a closer look into this set of equations. Clearly, in the pure s-wave limit, i.e., = 0, we reproduce our previous set of mean field equations in Eq. (4). In the pure d-wave limit, i.e., , becomes zero and we end with only the last two equations and it follows . Obviously this scenario is described in the case , where the electron band is incipient and . Since we choose large enough to make the solution energetically unfavorable we end up with the pure d-wave solution. However for we end up with finite and thus finite . For large enough , i.e., large enough , it is energetically unfavorable for the system to condense an additional d-wave component and thus . However, in between these two configurations we can end up in a state, where all five pairing amplitudes are finite. This set of equations is solved numerically in Fig. (8).

Similar to Section IV we obtain the equations of motion for this model by making use of Anderson pseudospin variables. The equations of motions have the same form as in Eq. (10) but the pseudo magnetic field is now , where we use and as introduced in the main text. Here, one needs to keep in mind that the electron order parameter has only the s-wave component, i.e., . The - and - component of the pseudo magnetic field are given by

 Δs,±h1(t)= −∑k[2UehS±ke(t)+Uhh,sS±kh2(t)] Δd,±h1(t)= −∑kUhh,dS±kh2(t)cos(2ϕk) Δs,±h2(t)= −∑k[2UehS±ke(t)+Uhh,sS±kh1(t)] (29) Δd,±h2(t)= −∑kUhh,dS±kh1(t)cos(2ϕk) Δ±e(t)= −∑k[UehS±kh1(t)+UehS±kh2(t)].

Including a time-dependent vector potential changes the pseudo magnetic field in the equations of motion into

 Blk=(−2Δxkl,−2Δykl,(ξk+ecA(t)l+ξk−ecA(t)l)). (30)

Choosing as in Eq. (16) we solve the equations of motion for a system inside the s+d regime numerically. Due to the momentum dependence of the order parameters the result is depending on the polarization of the vector potential. However, this does not change the qualitative dynamics. Similar to the s+s scenario we obtain that the dynamics of both - amplitude and relative phase oscillation - are clearly dominated by a single frequency . We find that all pairing amplitudes oscillate at the same frequency. While the relative phase between the hole order parameters remains constant for both s- and d-wave component, the relative phase between s- and d-wave component oscillate for each hole order parameter.
In Fig. (9) we investigate this frequency over the whole s+d phase diagram. We find that behaves similarly to the s+s scenario and vanished close to the borders of the s+d state. However, close to the border to the d-wave state one obtains that is coupling to , which can be understood as the system’s decreasing Higgs-mode due to the transition into the nodal d-wave state. This non-equilibrium effect is similar to the one observed in Ref. [31]. Once the collective mode of a system exceeds the system’s smallest possible Higgs-mode , this mode couples to and is therefore pushed below the quasiparticle continuum. The effect is not dominant on the border to the s-wave state, since the order parameter is fully gapped on this site.

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