Two-photon driven Kerr resonator for quantum annealing with three-dimensional circuit QED
We propose a realizable circuit QED architecture for engineering states of a superconducting resonator off-resonantly coupled to an ancillary superconducting qubit. The qubit-resonator dispersive interaction together with a microwave drive applied to the qubit gives rise to a Kerr resonator with two-photon driving that enables us to efficiently engineer the quantum state of the resonator such as generation of the Schrödinger cat states for resonator-based universal quantum computation. Moreover, the presented architecture is easily scalable for solving optimization problem mapped into the Ising spin glass model, and thus served as a platform for quantum annealing. Although various scalable architecture with superconducting qubits have been proposed for realizing quantum annealer, the existing annealers are currently limited to the coherent time of the qubits. Here, based on the protocol for realizing two-photon driven Kerr resonator in three-dimensional circuit QED (3D cQED), we propose a flexible and scalable hardware for implementing quantum annealer that combines the advantage of the long coherence times attainable in 3D cQED and the recently proposed resonator based Lechner-Hauke-Zoller (LHZ) scheme. In the proposed resonator based LHZ annealer, each spin is encoded in the subspace formed by two coherent state of 3D microwave superconducting resonator with opposite phase, and thus the fully-connected Ising model is mapped onto the network of the resonator with local tunable three-resonator interaction. This hardware architecture provides a promising physical platform for realizing quantum annealer with improved coherence.
The parametrically driven anharmonic oscillator, which is usually modeled by Kerr resonator with two-photon driving R1 (); R2 (), has been shown to display rich physics and thus has been studied extensively R3 (); R4 (); R5 (); R6 (); R7 (); R8 (); R9 (); R10 (); R11 (). In a system consisting of a Kerr resonator with two-photon driving operated in the quantum regime, where the Kerr nonlinearity is stronger than the photon decay rate, various schemes have been proposed for engineering the quantum state of the resonator R4 (); R6 (); R12 (); R13 (); R14 (). Among these efforts, preparing the Schrödinger cat state, i.e., superpositions of two large coherent states with opposite phases, has been extensively investigated for the development of quantum metrology R15 () and quantum information processing R15 (); R16 (). Moreover, driven by the pursuit towards practical quantum information processing, the quantum annealing R17 () was proposed as a quantum enhanced optimizer that aims to efficiently solve Ising problems R18 (); R19 (), and this resonator system has attracted increasing attention owing to its coupled network offering an new paradigm for quantum annealer R12 (); R20 (); R21 (); R22 (). In these paradigm, the quantum information is encoded and protected in the continuous variable system, i.e., resonator, and a series of theoretical studies have shown the robustness of these paradigm with respect to the dissipation and noise R21 (); R22 ().
Typically, the Kerr nonlinearity can be induced by inserting a nonlinear medium (Kerr medium) in a resonator. However, the induced Kerr nonlinearity is usually smaller than the dissipation rate in optical and mechanical systems, hindering the study of the quantum regime of this system. Recent advances in artificial solid-state system, especially in the cQED system, provides an alternative approach to easily get access to this fascinating quantum regimes R23 (). In the context of cQED, the Kerr resonator is realized by using a superconducting resonator with an embedded Josephson junction R24 (); R25 () which is almost an ideal non-dissipative nonlinear element R26 (). Therefore, this gives rise to two main approaches to realize the two-photon driven Kerr resonator in the cQED architecture. One approach to realizing the system is to use a superconducting coplanar resonator terminated by a flux-pumped SQUID R27 (); R28 (); R29 (). Alternatively, a recent experimental work has shown a nonlinear driven-dissipation approach by using a 3D microwave resonator coupled to fixed-frequency transmon qubit and by an external microwave drive applied to the qubit at the resonator frequency R30 (). For the latter approach, remarkably, the 3D microwave resonator with high quality factors has been experimentally demonstrated R31 (), enabling storage times approaching seconds R32 () and thus favoring the quantum information processing based on the 3D microwave superconducting resonator R16 (); R33 (). However, it is noted that this approach is implemented by using the two-photon driven-dissipation process where the engineered nonlinear (two-photon) decay rate should be significantly larger than the single-photon decay rate of the cavity, which still remains important challenges to be overcome R30 (). This current limitation suggests investigating another relatively easily realizable approach that also exploits the large coherence times of the 3D microwave superconducting resonator.
In this work we proposed an experimentally feasible protocol for realizing two-photon driven Kerr resonator in a cQED architecture, which, in principle, is compatible with the 3D cQED architecture with high coherence. The Kerr resonator with two-photon driving, which lie at its heart, is realized via off-resonantly coupling a resonator to an ancillary microwave-driven superconducting qubit. In our setting, the superconducting qubit is treated as a quantum three-level system that is initially in its ground state, and remains unexcited in the whole process, minimizing the effect of the qubit decoherence. Moreover, based on our protocol for realizing two-photon driven Kerr resonator, we apply a combination of the recently proposed resonator based LHZ annealer R21 () and the 3D cQED architecture that allows a flexible and scalable hardware architecture with long coherence times for LHZ annealer. In our setting, each spin in the LHZ represented Ising problem is encoded in the degenerate ground subspace of the two-photon driven Kerr resonator formed by two coherent states of opposite phases, and the four-body constraints, which are decomposed into two three-body constraints, are physical implemented with the use of a transmon qubit mediated tunable three-resonator interactions.
Ii the system and Hamiltonian
In order to construct a circuit-QED platform for engineering quantum state of resonator, and further implementing the quantum annealing, here we introduce two major ingredients, two-photon driven Kerr resonator, which allows us to create non-classical state of resonator such as Schrödinger cat states, and the tunable resonance three-resonator interaction. Meanwhile, we also aim to exploit the long coherence of the 3D superconducting resonator, thus the presented platform should be compatible with the 3D architecture. With these aims in mind, in the following discussion: (i) We propose a scheme to realize the two-photon driven Kerr resonator in a qubit-resonator system, where the resonator is coupled to a superconducting qubit and the qubit is driven by a coherent microwave drive applied at well-chosen frequency, as shown in Fig.1. (ii) We show that a tunable resonance three-resonator interaction can be induced by coupling resonators to a transmon qubit, where the qubit mode decouples form these resonator modes and mediates the three-resonator interaction by applying a suitable pump mode on it, as shown in Fig.3. In doing so, we present a thorough description of the two ingredients for the coupled network of two-photon driven Kerr resonators. We now turn to present the quantitatively derivation.
ii.1 Kerr-nonlinear resonator with two-photon driving
As shown in Fig.1(a), we consider a system consisting of a resonator coupled to a quantum three-level system (qutrit), for which the transitions and of the qutrit are off-resonantly coupled with the resonator, while the transition is coupled to a coherent microwave drive with a frequency at the nearly twice the resonator frequency. The proposed scheme can be physically realized in a circuit QED architecture consisting of a superconducting resonator capacitively coupled to a superconducting qubit, which can be realized by using flux qubit R37 (); R38 () or fluxoninum qubit R39 (), as depicted in Fig.1(b). Here, we focus on the lowest three energy levels of the superconducting qubit and thus we treat the qubit as a three-level system (qutrit) (see Appendix A for details of the circuit-QED system). After applying the rotating wave approximation (RWA), the full system can be described by the Hamiltonian (, throughout the paper)
describes the free Hamiltonian of the resonator and the qutrit,
describes the qutrit-resonator interaction, and
describes the time-dependent drive of the qutrit. Above, , are the creation and annihilation operators for the resonator of frequency . is the transition frequency of the qutrit from ground to excited state . and denote the qutrit-resonator coupling strength, and is the real amplitude of the microwave drives at frequency . For simplicity, we define in the following discussion.
We consider that our system operates in the dispersive regime, where the qutrit is far detuned from the resonator , and also the microwave drive . In this situation, the systemic Hamiltonian can be well approximated by the effective Hamiltonian R40 (); R41 (); R42 ()
where is the renormalized resonator frequency
The second term denotes the qutrit-induced self-Kerr-nonlinearity of the resonator with
The last term represents a two-photon drive of amplitude
applied on the resonator at frequency .
In deriving Eq.(5), it is worth mentioning that: (i) We have also assumed that the qutrit is initially in its ground state. As the qutrit-resonator system operates in the far-detuned dispersive regime, no energy is exchanged between the field mode (resonator and the microwave field) and the qutrit, thus the qutrit remains unexcited. Therefore, one can eliminate the degrees of freedom of the qutrit and the effective Hamiltonian is obtained. (ii) For a realistic implementation depicted in Fig.1(b), we have ignored several terms due to their negligible effects, the highly off-resonance coupling between transitions (i.e, , ) and the qutrit drives. For clarity, we have also omitted the term describing the coupling between qutrit transition and resonator in the Hamiltonian in Eq.(1). However, this does not alter the main result except making another contributions to the coefficient and , see Appendix A for the complete derivation. Moreover, these terms are taken into account in the following numerical analysis.
As a result, we have demonstrated that the qutrit-resonator system depicted in Fig.1 can be modeled as a two-photon driven Kerr resonator. Recent theoretical studies have shown that the schrödinger cat state can be generated via quantum adiabatic evolution of the system described by the Hamiltonian Eq.(5) R12 (); R13 (). This can be made clear by moving to a rotating frame with respect to such that the Hamiltonian Eq.(5) is simplified to R13 ()
For simplicity, we assume that and are positive for the following discussion. It is apparent that the ground state is two-fold degenerate. The coherent states , are the degenerate eigenstates with energy , and thus also the schrödinger cat states
where the is the normalizing factor, and the label the even- and odd cat-states, respectively. Moreover, the vacuum state and the one-photon Fock state are also the ground eigenstates with even and odd parity for the undriven case (). As the Hamiltonian preserves the parity, when one gradually increases the amplitude of the two-photon drive , the driven system will evolve adiabatically along two paths with for the system initially prepared in the vacuum state and single-photon Fock state, respectively R12 (); R13 ().
To show the validity of our proposal for the two-photon driven Kerr resonator, we present in Fig.2 the numerical analysis of the time evolution of the qutrit-resonator system, initially in , with a microwave drive applied on the qutrit R13 () (see Appendix B). The total evolution time and are chosen to satisfy the adiabatic condition, and we use s and s in this work. Parameters used in the numerical simulation are GHz, GHz, GHz, GHz, GHz, and GHz, yielding MHz. For the microwave drive with different amplitude (i.e., GHz), Figure2(a)-(d) show the Wigner function for the resonator at the end of the adiabatic evolution, respectively, and the resonator evolves to the even cat state as we expected. The time evolution of the average photon number in resonator is also displayed in the upper panel of Fig.2(e), and the photon number at time shows good agreement with the value calculated by , yielding the average photon number for the four different drive amplitudes, respectively.
The lower panel of Figure2(e) shows the population leakage to the excited state of the qutrit, where the diamond-markered line and circle-markered line represent the leakage to and , respectively, which leads to an important limitation of our proposal for larger drive amplitudes. These results show that for the fixed system parameter, increasing will increase the population leakage, causing undesirable entanglement of the resonator and qutrit and adding another decay channel of the resonator. Figure2(f) shows the time dependent of the fidelity of the cat state , in which , and is the reduced density matrix of the resonator. The markered line represents the time evolution of the fidelity without the effect of dissipation, while the solid line corresponds to the situation by considering the effect of photon decay and qutrit relaxation. As we expected, increasing the microwave drive amplitude will increase the infidelity. Meanwhile, the infidelity caused by these population leakage can be made smaller by increasing the qutrit-resonator detuning. However, we note that increasing the qutrit-resonator detuning would entail a sacrifice of the magnitude of the Kerr nonlinearity and the two-photon drive.
ii.2 Tunable resonant interactions among three resonators
Here, we present a scheme for realizing tunable three-resonator interaction and the interaction of interest to us is
where the and are the creation and annihilation operators for the th resonator of frequency . As shown in Fig.3, we consider a system consisting of three strongly detuned resonators dispersively coupled to a transmon qubit. With the nonlinear cosine-coupling contributing from the Josephson junction of the transmon qubit, four-wave mixing processes that conserve energy, can happen by applying a suitable pump mode on the qubit. Similar process have been experimentally demonstrated in 3D cQED architecture R30 (); R43 (); R43 (). Here, we looks for a four-wave mixing process, where a pump photon in combination with a resonator photon (with frequency ) can create a photon in both the other two resonators at frequencies and , respectively, that results the three-body interaction described by the interaction Hamiltonian given in Eq.(11).
Now, we turn to give a quantitatively derivation of the effective Hamiltonian. The Hamiltonian of the system depicted in Fig.3 is R30 ()
where and () are the creation and annihilation operators for the th mode with bare frequency , and is Josephson energy of the qubit mode. is the phase difference across the junction, and () is the zero-point fluctuation of flux associated with the th mode. The term in the second line of Eq.(12) describes a pump mode with real amplitude applied on the qubit mode at frequency .
In order to see clearly how the four-wave mixing process can lead to the desired three-resonator interaction, it is helpful to move to a displaced frame by performing a time-dependent transformation with and on the above Hamiltonian R30 (). Assuming small phase fluctuations, we can expand the cosine up to the fourth order, and the resulting Hamiltonian after a rotating wave approximation in the displaced frame reads (see Appendix C for more details)
where is the frequency for the th mode including a renormalization of the transition frequency coming from the qubit-resonator coupling and the pump mode induced AC Stark shift. is the three-body coupling strength, which can be controlled by the pump drive. When the pump frequency matches the detuning of the three resonators, i.e., , the interaction Hamiltonian given in Eq.(11) is obtained. Moreover, by tuning the magnitude and the phase of the pump drive, one can realize an amplitude- and phase-tunable three-resonator interaction, which is useful to implement the ramp protocol for quantum annealing, as we demonstrated in the following section.
Iii resonator based Lechner-Hauke-Zoller annealer with three-body constraints
In this section, we show that our procedure to realize the two-photon driven Kerr resonator and the tunable resonance three-resonator interaction in the circuit-QED architecture, as demonstrated in Sec.II, could be used for the implementation of quantum annealing with LHZ scheme.
Here, for easy reference and to set the notation, we briefly review some basic concepts of quantum annealing and also the LHZ scheme. The quantum annealing was proposed as a quantum enhanced optimizer that aims to efficiently solve optimization problems. In quantum annealing, one can map an optimization problem into the all-to-all Ising spin glass model R45 ()
where is the Pauli operator for the th spin. The local field and the strength of the spin-spin coupling fully define the optimization problem. The solution of the optimal problem now amounts to finding the ground state of the Ising spin glass model (Ising problem), and this can be achieved by executing the time-dependent Hamiltonian
where is the initial Hamiltonian with a trivial ground state (e.g., ) and is the total evolution time. For a system, which is governed by the Hamiltonian and initially in its ground state, evolving adiabatically, the system will stay in the instantaneous ground state of the Hamiltonian at each time . Therefore, at the end of the evolution , the system will stay in the ground state of , which encodes the desired solution of the optimal problem.
However, to solve a practical optimal problem mapped into the Ising model with full connectivity, one leading physical restriction that makes the direct physical implementation of the model becomes untractable is that interactions between physical systems are commonly local, which favors local interaction between spins rather than long range interaction. To get ride of this obstacle, an embedding technique, now known as minor embedding scheme, was first introduced R46 (); R47 (). Recently, Lechner et al. R34 () proposed an alternative embedding scheme in which the full connected Ising model with logical spins [Fig.4(a)] is encoded in physical spins with local constraints in a triangular lattice, as shown in Fig.4(b) R48 (). In the LHZ scheme, each physical spin encodes the relative orientation of the corresponding pair of logical spins, i.e., the physical spin take and for aligned (i.e., , ) and antialigned (i.e., , ) logical pair, respectively. Meanwhile, the local constraints are introduced for suppressing the redundancy of the encoding scheme. With this scheme, only local four-body terms and programmable local fields applied on the physical spin are needed R49 (). These features along with the potential of scaling up make it attractive for practical physical implementation, and various physical implementation scheme have been proposed R21 (); R35 (); R36 (); R50 () and demonstrated experimentally for small system R51 (). In particular, the resonator-based implementation proposed in Ref. has been shown to be realizable and noise-resilient. Therefore, in the following discussion, by combining the advantage of this resonator-based implementation and the long coherence times attainable in 3D cQED, we propose a scalable hardware for implementing resonator-based LHZ annealer with three-body constraints, which is compatible with 3D cQED architecture.
iii.1 the Lechner-Hauke-Zoller scheme with three-body constraints
In the LHZ scheme, each four-body constraint can be realized directly by using a four-spin interaction , in which the , , , and label the physical spin involved in the th four-body constraint, and the interaction strength should be the dominant energy scale in the embedding model R34 (); R36 (). Therefore, for a physical implementation of the LHZ scheme with four-body constraints, the Ising problem Hamiltonian reads R34 ()
with logical field acted on the th physical spin and the magnitude of the four-spin coupling strength.
However, the four-spin interaction is still hard to be physically realized with considerably high coupling strength. Recently, Leib et al. R35 () have theoretically demonstrated that one can use a general recursive decomposition of classical k-local Ising terms, decomposing the four-body constraints into two three-body constraints,
with an ancillary physical spin labeled by . It is noted here that each ancillary physical spin does not encode any information of the logical spin configuration, but mediates the three-body realization of the four-body constraints. Therefore, one can realize the LHZ scheme with three-body constraints, which can be realized directly by using a three-body interaction . For a physical implementation of the LHZ scheme with three-body constraints, the Ising problem Hamiltonian becomes
with , and .
In order to evaluate the performance of the LHZ scheme with three-spin interactions, we present in Fig.5 the time-dependent energy spectrum of the executing Hamiltonian for the Ising problem with logical spins, and the Ising problem Hamiltonian are represented by Eq.(14), Eq.(16), and Eq.(18), respectively. In the numerical simulation, we consider that the initial Hamiltonian is given as with , and we use the local field strength , spin-spin coupling strength that is randomly taking from the interval , and the constraints strength . As shown in Fig.5, although different trajectories of the time-dependent spectrum have been shown for the three schemes, an almost perfect agreement of the lower energy levels is displayed at time , demonstrating preliminarily the validity of the three-body constraints implementation of the Ising problem.
In the practical quantum annealing process, the minimal gap is the leading limitation restricting the sweep time and also the main source of errors in quantum annealing, i.e., Landau-Zener transitions. For the LHZ scheme with three-body- and four-body constraints, we further presents in Fig.6(a) the comparison of the minimal gap. For random instances, the three-body constraints based implementation does not considerably decrease the minimal gap, and even the two implementations show a similar result for four different constraint strengths ().
Alternatively, compared with the ramp protocol described by the Hamiltonian Eq.(15) where in the annealing process, the constraint terms are adiabatically changed form to , it is also possible to use an always-on protocol (i.e., the strength of the constraints are fixed in the whole process). Using this always-on protocol, the Ising problem encoded by the LHZ scheme is fully characterized by the local fields applied on the physical spin, and thus one can simplify the physical system and reduce the complexity for quantum annealing. Recent theoretical studies have demonstrated that the gap in the always-on protocol is in general smaller, but with only a small systematic difference between the two in favor of the ramp protocol R35 (). However, as shown in Fig.6(b), the minimal gap in the three-body implementation with ramp protocol is general larger than the one in the four-body always-on protocol . This suggests that the three-body implementation with ramp protocol may have better performance than the four-body always-on protocol. In the following discussion, we propose a resonator based system for implementing the LHZ scheme with three-body constraints, and the tunable three-body interactions in the proposed system allows for ramp protocol.
iii.2 The coupled network with application to the Lechner-Hauke-Zoller annealer
Following the recent theoretical studies in Ref., here we show that the cQED architecture proposed in Sec.II, can be used to realize the LHZ scheme with three-body constraints, where the spin states are encoded in the degenerate ground subspace of the two-photon driven Kerr resonator formed by two coherent states of opposite phases, i.e, , respectively, and the three-body constraints are directly implemented with three-resonator interactions mediated by the transmon qubit, as we introduced in Sec.II(B). Moreover, the proposal allows tunable three-resonator interactions that enables the ramp protocol for the LHZ annealer.
For the triangular network as shown in Fig.4(b), we consider that each spin is physically realized by a two-photon driven Kerr Resonator, and all the four-body constraints are physically realized by two three-resonator interactions with an ancillary resonator, as shown in Fig.4(d), while the three-body constraints in the base of the lattice is directly realized by three-resonator interactions. Meanwhile, the local field acted on the physical spin is introduced by a single-photon drive applied on the resonator R20 (); R21 (). To implement the adiabatic ramp protocol for a general -spin Ising problem with the proposed triangular network, the executing time-dependent Hamiltonian reads (in the lab frame)
describes the th resonator with self-Kerr coefficient and a two-photon drive of amplitude at frequency , similar to the one given in Sec.II(A),
represents the additional single-photon drive of amplitude applied on the th resonator at frequency , and
denotes the three-resonator interaction with strength , which is induced by a pump mode at frequency , as demonstrated in Sec.II(B).
In a frame where each of the resonator rotate at the instantaneous single-photon drive frequency, i.e., applying the unitary transformation on above expression, the Hamiltonian now reads R21 ()
acts as the initial Hamiltonian for implementing quantum annealing, whose ground state is vacuum state that is actually simpler to be prepared, and
characterizes the Ising problem by using the LHZ scheme with three-body constraints. The correspondence between the above expression and the Hamiltonian given in Eq.(18), can be found directly by projecting Eq.(25) on the tensor product (i.e., ) of the spaces spanned by , where the is real number, and by dropping constant terms, resulting
with and . However, as mentioned in Ref. and demonstrated in Refs.[13, 21], the above procedure is valid only if the single-photon driven strength is sufficiently smaller, and also the three-resonator coupling strength .
To give a preliminary verification of the above resonator based LHZ annealer, we present in Fig.7 the time-dependent energy spectrum of the Hamiltonian in Eq.(15) and Eq.(25), respectively, with . At the end of the evolution , an almost perfect agreement of the lower energy levels is displayed. Furthermore, in the left panel of Fig.(7), we present the the spin configuration of the ground state of Ising problem described by Eq.(15) with different parameters, resulting for (a)-(d), respectively. We also show, in the right panel, the ground state of the corresponding resonator-based LHZ annealer at time , where the state of the first two resonators reproduces the spin configuration of the ground state of the Ising problem, while the state of the third resonator confirms the relative orientation of the two logical spins. The whole fidelity , in which , is the sign of the amplitude of the th resonator for an ideal encoding, and is the eigenstate of the executing Hamiltonian Eq.(23) at , are for the four different spin configurations, respectively.
In conclusion, we propose a new scheme for implementing two-photon driven Kerr resonator in a cQED architecture consisting of a superconducitng resonator capacitively coupled to a microwave driven superconducting qubit, and by using realistic parameters, we show that the Schrödinger cat state can be prepared via adiabatic evolution in the microwave-driven qubit-resonator system. Contrary to the implementation by using superconducting coplanar resonator terminated by a flux-pumped SQUID, our protocol is compatible with the 3D architecture that allows us to exploits the large coherence times of the 3D microwave superconducting resonator. The major limitation of our proposal is the population leakage for lager drive amplitudes, which results infidelity, and in principle, this can be further decreased by looking for optimal parameter set of the qubit-resonator system. As a possible extension, one may also apply this protocol to a hybrid quantum system consisting of a spin or atomic ensemble coupled to a superconducting circuits R53 (), allowing generation of spin (atomic) Schrödinger cat state and spin squeezing for quantum enhanced sensing and metrology R54 (); R55 ().
Inspired by the recent theoretical work, we further show that the presented architecture to realize two-photon driven Kerr resonator together with the introduced tunable three-resonator interaction, can be scaled easily up to a coupled network for the implementation of resonator based LHZ annealer. The tunable three-resonator interaction allows for the ramp protocol of our quantum annealer. Therefore, comparing with the always-on protocol, our implementation with ramp protocol may have better performance. Furthermore, in principle, the annealer that we have proposed can be realized in the 3D cQED architecture R56 (); R57 (), for which the coherence times of the 3D microwave superconducting resoantor can exceed that of the best superconducting qubit by almost two orders of magnitude R31 (); R32 (). This makes our proposed implementation a promising physical platform for realizing quantum annealer with improved coherence.
Acknowledgements.We thank Chui-Ping Yang for useful discussions. Thanks also to the developers of the PYTHON package QuTiP R58 (); R59 (), which was used for numerical calculation. This work was partly supported by the NKRDP of China (Grant No. 2016YFA0301802) and NSFC (Grants No. 11504165, No. 11474152, and No. 61521001).
Appendix A The realistic circuit-QED implementation
Figure 8 shows the circuit model of the capacitively-shunted flux qubit (C-shunt flux qubit) R60 (); R61 (), which is capacitively coupled to an LC resonator R61 (); R62 (); R63 (). The two identical Josephson junctions have capacitance and coupling energy , while the third (smaller one) has capacitance and coupling energy . and represent the equivalent inductance and capacitance of the resonator, respectively. represents the coupling capacitance between the resonator and the flux qubit, for which the smaller junction is shunted by a capacitance . In the following discussion, the phase difference across the larger Josephson junctions and the inductance are denoted as and , respectively. The Lagrangian of the system is given by
where , and with , where is the externally applied magnetic flux in the loop. For clarity, this equation can be rewritten as
with . Following the procedure of Ref., the system can described by a Hamiltonian consisting of three parts,
is the qubit Hamiltonian,
is the resonator Hamiltonian, and
is the qubit-resonator interaction Hamiltonian. Above, and are the creation and annihilation operators for the resonator with frequency
and , , , and are conjugate variable of the phase differences .
According to the parameters listed in Table 1, Figure 9 shows the energy spectrum of the flux qubit from the ground state and the coupling strength , where represents the th eigenstate of the uncoupled qubit Hamiltonian given in Eq.(A4), as a function of the flux bias .
In this work, we focus on the lowest three energy levels of the flux qubit and thus in this situation the flux qubit is considered to be a perfect three-level system (qutrit). After using the RWA, the Hamiltonian of the qutrit-resonator system is
By introducing a microwave drive tone applied on the qutrit, the full system Hamiltonian reads
here stands for Hermitian conjugate, and is the transition frequency of the qutrit from ground to excited state . , , and denote the qutrit-resonator coupling strength. is the real amplitude of the microwave drive with frequency applied to the transition of the qutrit. For simplicity, we define in the following discussion.
We consider that our system operates in the dispersive regime, where the qutrit is detuned from the resonator , and the qutrit is off-resonantly driven by the microwave drive . Moreover, we suppose that the qutrit is initially in its ground state. Therefore, the qutrit remains unexcited in the process and thus decouples from the resonator. In these conditions, by using the fourth-order perturbation theory R40 (); R64 (), and eliminating the degrees of freedom of the qutrit, the Hamiltonian in Eq.(A9) can be well approximated by the effective hamiltonian
where is dressed resonator frequency with
The second term denotes the qutrit-induced Kerr-nonlinearity of the resonator with
The last term represents a two-photon drive of amplitude
applied on the resonator at frequency .
Appendix B master equation
The influence of photon decay and qubit relaxation on the quantum adiabatic evolution can be studied by the master equation approach. By including photon decay and qubit relaxation terms, we can write the master equation R65 ()
Above, is the density matrix of the entire system, is the Hamiltonian of the full system given in Eq.(A9), and is the Lindbladian of the operator . and denote the photon decay rate of the resonator and the relaxation rate of the two level systems, respectively.
To make a direct comparison of the evolution of the effective model describing by Hamiltonian in Eq.(9) in the main text and that of our proposed full microwave-driven qutrit-resonator system describing by the Hamiltonian in Eq.(A9), it is helpful to move to the rotating frame corresponds to the interaction picture with respect to the renormalized frequency of the resonator, that is the change of variables in Eq.(B1)
In this new frame, the master equation is given as