Universal holonomic quantum gates in decoherence-free subspace on superconducting circuits

Universal holonomic quantum gates in decoherence-free subspace on superconducting circuits

Zheng-Yuan Xue zyxue@scnu.edu.cn Guangdong Provincial Key Laboratory of Quantum Engineering and Quantum Materials, and School of Physics
and Telecommunication Engineering, South China Normal University, Guangzhou 510006, China
   Jian Zhou Guangdong Provincial Key Laboratory of Quantum Engineering and Quantum Materials, and School of Physics
and Telecommunication Engineering, South China Normal University, Guangzhou 510006, China
National Laboratory of Solid State Microstructure, Nanjing University, Nanjing 210093, China
   Z. D. Wang Department of Physics and Center of Theoretical and Computational Physics, The University of Hong Kong,
Pokfulam Road, Hong Kong, China
July 15, 2019

To implement a set of universal quantum logic gates based on non-Abelian geometric phases, it is a conventional wisdom that quantum systems beyond two levels are required, which is extremely difficult to fulfill for superconducting qubits and appears to be a main reason why only single-qubit gates were implemented in a recent experiment [A. A. Abdumalikov Jr. et al., Nature (London) 496, 482 (2013)]. Here we propose to realize nonadiabatic holonomic quantum computation in decoherence-free subspace on circuit QED, where one can use only the two levels in transmon qubits, a usual interaction, and a minimal resource for the decoherence-free subspace encoding. In particular, our scheme not only overcomes the difficulties encountered in previous studies, but also can still achieve considerably large effective coupling strength, such that high fidelity quantum gates can be achieved. Therefore, the present scheme makes realizing robust holonomic quantum computation with superconducting circuits very promising.

03.67.Lx, 42.50.Dv, 85.25.Cp

I Introduction

Under adiabatic cyclical evolution, a quantum system acquires a phase factor, which consists of both dynamical and geometric components. When the eigenstates of the system are nondegenerate, the geometric component is the well-known Berry phase berry (). For the degenerate case, it is a unitary operator acting on the degenerate subspace, i.e., holonomy wz (). As geometric phases are determined by the global property of the evolution path, the geometric method of quantum computation has been shown to possess some built-in noise-resilience features exp1 (); exp2 (); exp3 (); exp4 (); exp5 (); exp6 (); zhunoise (); noise (). In general, the holonomies do not commute with each other, and thus can be used to construct a universal set of quantum gates h (); h1 (); h2 (); h3 (); h4 (); h5 (); zp (); oo (); h6 (); h7 (); h8 (); h9 (); h10 (), i.e., the holonomic quantum computation (HQC).

On the other hand, the adiabatic method of quantum computation intrinsically leads to long gate operation time, which may be comparable with the lifetime of typical qubits xbw (); zhuspeed (). This motivates research on quantum computation based on the nonadiabatic geometric phases. Recently, nonadiabatic HQC has been proposed using three-level systems n1 () with the experimental implementation of some elementary gates e1 (); e2 (); e3 (); e4 (). However, the excited state is resonantly coupled when implementing the quantum gates n1 (), and thus, its limited lifetime is a main challenge in practical experiments. Note that this limitation may be avoided in experiments in Refs. e3 () and e4 () because they use the three magnetic states of a nitrogen-vacancy center in a diamond. However, for a superconducting transmon qubit, this limitation does exist, and recent experiment has verified only single-qubit gates e2 (). The energy levels of a transmon qubit transmon () are in a ladder shape, and the anharmonicity is small, which limits the coupling strength between neighboring levels to the order of 10 MHz in order to individually address the interactions e2 (); supertime (). Therefore, even with newly demonstrated good coherent times of multilevels in the transmon qubit supertime (), the implementation of a nontrivial two-qubit holonomic gate, which needs much more complicated cavity-induced interaction between two three-level systems n1 (), is still very challenging. Alternatively, there are schemes using circuits more complicated than transmons to mimic a multilevel system exp5 (); h5 (); h7 (). However, this will inevitably introduce additional noises from the environment because more circuits and control elements are needed.

Meanwhile, many efforts have also been made to combine HQC with the decoherence-free subspace (DFS) encoding dfs1 (); dfs2 (); dfs3 (). HQC in DFS law (); n2 (); n3 (); n4 (); n42 (); n5 () can consolidate both the noise resilience of the encoding and the operational robustness of holonomies. As for transmon qubits, this protocol is much more difficult to implement because it requires at least two transmon qubits to encode a logical qubit, and thus, more complex interactions among qubits are needed, even in the single-qubit-gate case. Moreover, previously proposed schemes based on HQC in DFS usually need at least three physical qubits to encode a logical qubit; note that the use of two physical qubits is a minimum resource needed, as in Ref. xlf () for geometric entangling gates.

In this paper, we propose to implement a nonadiabatic HQC in DFS with a typical circuit QED setup. Our scheme avoids the above-mentioned difficulties. First, only the two energy levels of the transmon qubits are involved. Second, for the single-qubit case, our implementation relies solely on the effective resonate qubit-cavity interaction. Meanwhile, for the two-qubit case, only a conventional detuned interaction is required, where the detuning between a transmon qubit and the cavity is fixed, and thus, we have plenty freedom to avoid the limitation due to the small anharmonicity of transmons. Third, we use two transmons to encode a logical qubit, which is the minimal resource for the DFS encoding. Therefore, our scheme presents a promising method for HQC on superconducting circuits.

Figure 1: (Color online) Illustration of the setup of our scheme. (a) The coupled two-transmission-line-resonator system for universal holonomic quantum computation in a decoherence-free subspace, in which each resonator has two transmon qubits to encode a logical qubit. (b) The qubit and cavity coupling configuration.

Ii The setup and interaction

The setup we consider is illustrated in Fig. 1(a), which consists of two coupled transmission line resonators (one-dimensional cavities). In each cavity, there are two transmon qubits transmon () capacitively coupled to it. This coupled system is the building block of our scheme, and the two transmon qubits encode a logical qubit. For the case of single-logical-qubit gates, we consider only the dynamics within a cavity, while the coupling between the two cavities is switched on when implementing the two-logical-qubit gate. Furthermore, one may repeat this block to construct a one-dimensional chain of logical qubits; that is all the parameters of the odd and even qubits are the same as those of the first and second qubits, respectively.

We first detail our setup for the single-qubit case. A transmon qubit is composed of two identical Josephson junctions in a loop configuration and is shunted by a large capacitance. The transmon qubit is quantized and its lowest two energy levels can be used to construct our physical qubit states with the effective Hamiltonian (), where is the energy splitting of the transmon qubit and is the Pauli matrix of the th transmon qubit in its eigenbasis. For typical values of experimental parameters, GHz cqed (). The transmon qubits are located at the voltage antinodes of the relevant cavity mode, , where , , and are the frequency, annihilation, and creation operators of the cavity, respectively. The coupled system is described by cqed ()


where is the qubit-cavity coupling strength (assumed to be real), is the transmon lower operator, and . Here we consider the case of ; that is, the qubit-photon interaction acts perturbatively.

To get a resonate interaction between a selected transmon qubit and the cavity, the qubit is biased by an ac magnetic flux, which will introduce periodical modulation eff () of the qubit transition frequency in the form of


This modulation may effectively turn the qubit’s sideband on resonance with the cavity frequency. This can be clearly seen by moving to the rotating frame defined by ,


with , and the transformed Hamiltonian is

Using the Jacobi-Anger identity of

and , with being Bessel functions of the first kind, the transformed Hamiltonian reduces to

When , the effective resonate qubit-cavity interaction will be in the form of


where , we have applied the rotating-wave approximation by neglecting the oscillating terms, and the smallest oscillating frequency is , i.e.,

In this way, we can have full control of the coupling strength by varying the externally driven ac magnetic flux, i.e., by controlling the amplitude and phase . Meanwhile, assuming that the anharmonicity of the transmon is the same as , as the transition frequency of is , the third level of the transmon can only couple dispersively with the detuning , as shown in Fig. 1(b). Finally, note that the resonate interaction in Eq. (6), for the case with more than two qubits, has the conserved quantity of total excitation , with being the photon number in the cavity.

Iii Single qubit gates

We now proceed to deal with the holonomies for single-qubit gates in DFS. Hereafter, to avoid confusion, we refer to our physical transmon qubits as transmons and logical qubits as qubits for short. As the transmons are placed in the same cavity, they can be treated as interacting with the same cavity-induced dephasing environment. The DFS we consider here is the subspace of


where the subscript denotes the states belonging to the logical qubit and , i.e., they denote the states of the first and second transmons, and the cavity, respectively. Also, we use the cavity as an ancillary, and thus, only two transmons are needed to encode a logical qubit. Note that the DFS is identical to the subspace of , which ensures that the quantum dynamics will not go out of subspace .

In this encoding, the Hamiltonian of the quantum system consisting of two transmons, i.e., , resonantly coupled to a cavity reduces to


where is the effective Rabi frequency, , and . In this case, we construct a -type Hamiltonian in the DFS with only resonate transmon-cavity interaction, from which an arbitrary single-qubit holonomic gate can be obtained. It is worth pointing out that the two transmons do not have to possess the same frequency, as we may use two externally driven fields with different frequencies to bring them in resonance with the cavity.

In the dressed-state representation, the Hamiltonian in Eq. (9) can be viewed as indicating that state couples with only the ”bright” state , while it decouples from the ”dark” state . Under the action of , the dark and bright states evolve according to


When the condition is satisfied, the dressed states undergo a cyclic evolution as . Under this condition, the time evolution operation on the subspace {} is given by


where is the time-ordering operator and . In particular, when the condition is met, which means that there is no transition between the two time-dependent states, the evolution satisfies the parallel-transport condition. Therefore, the geometric nature of the operation is originated from the structure of the Hamiltonian instead of the slow evolution in the adiabatic case. Under these two conditions, in the logical qubit subspace , the nonadiabatic holonomic gates can be realized as


where and can be tuned by choosing approximate parameters of the externally driven ac magnetic fluxes. Therefore, an arbitrary single-qubit gate can be achieved.

Figure 2: (Color online) The performance of the proposed Hadamard gate. (a) Qubit-state population and fidelity dynamics of the Hadamard gate as a function of dimensionless time . (b) Maximum fidelity for different cavity decay rates (in units of ) and , with being 50 and 100 MHz for the blue circles and red triangles, respectively.

The performance of the gates can be evaluated by considering the influence of dissipation using the quantum master equation:


where is the density matrix of the considered system; is the Lindblad operator; and , and are the decay rate of the cavity and the decay and dephasing rates of the qubits, respectively. We have assumed that the decay and the dephasing rates of the two transmons are the same. We consider the Hadamard gate to be a typical example, where and . To make the total coupling strong, we may choose and , which corresponds to . This can be achieved by modulating and ; note that tuning the coupling strength in such a way has been experimentally demonstrated eff (). We may choose MHz, MHz, and thus MHz. To verify the approximation when obtaining Eq. (6), we also include some oscillating terms in the simulation. As , the term can be safely neglected for transmon 1. Meanwhile, for transmon 2, this ratio is also larger than 4. Therefore, for demonstration purposes, we include only the terms in Eq. (II) for the two transmons in our numerical simulation, i.e., in Eq. (13),


Quality factors of about have been reported for a cavity with frequencies ranging from 4 to 8 GHz cavitydecay (), and thus, the cavity decay rate is on the order of kilohertz. Relaxation and coherence times of 44 and 20 s are reported qubitdecay () for a planar transmon, which corresponds to kHz and kHz. As , and are all on the same order of magnitude, for simplicity, we treat them as if they were identical and set kHz. Suppose the qubit is initially in the state ; we evaluate this gate by the qubit-state population and the fidelity defined by , with being the ideally final state under the Hadamard gate. We solve numerically the master equation (13) with being given in Eq. (II); as shown in Fig. 2(a), we obtain a very high fidelity at ns. Meanwhile, the higher energy levels will also be involved during the evolution; we next consider the effect of the third level of the transmons, which is the one closest to . Note that more higher excited levels will not directly influence the transmon qubit subspace. For this level, we assume that the anharmonicity of the transmon is the same as , and thus, the cavity-induced coupling between the second and third levels when obtaining the Hamiltonian in Eq. (6) is dispersive, i.e., oscillating with frequency . Therefore, its contribution to the infidelity of the quantum gates is similar to that of the Hamiltonian in Eq. (II). Assuming that the coupling strength is , the infidelity that results from this third level is from our numerical simulation. In addition, when the transmons are incorporated into the cavity, its decay rate will be enhanced. Therefore, we also investigate the influence of the increase of the cavity decay on the gate fidelity; as shown by the blue circles in Fig. 2(b), for , we can still get . Meanwhile, the larger detuning implies can be bigger, and thus, the fidelity can be higher. As shown by the red triangles in Fig. 2(b), we verify this by choosing the detuning and transmon-cavity coupling strength to be 2 and 2, respectively.

Iv Two-qubit gate

At this stage, we turn to the implementation of a nontrivial two-qubit gate. To avoid the cross talk between transmons, we consider the scenario of two coupled cavities, with each one having two transmons to encode the logical qubit. In this case, a six-dimensional DFS exists


where ; and are two ancillary states, both of which have two excitations within a logical qubit and thus will not be affected in the single-qubit cases (in the subspace).

To obtain a nontrivial two-qubit gate, we need to induce the interaction within two transmon pairs, i.e., transmons 2 and 3 and transmons 2 and 4, but to avoid the interaction between other pairs. To achieve this, we consider that the interaction is induced by exchanging virtual photons between the two coupled cavities, the coupling of which is cc ()


and the frequencies of the delocalized field modes and are shifted dyn () from the bare cavity frequency as and , respectively. In addition, to avoid cross talk between the two interacting pairs, they have different detunings. The setup is detailed as follows. For transmons 3 and 4, which are located in the second cavity, we do not apply externally driven on them and set MHz, MHz, and . As for the third energy level, the anharmonicity of the transmon is approximately MHz, and thus, the higher levels can be safely neglected. Then, in the bare cavity frequency, the interaction Hamiltonian reads


Meanwhile, for transmon 2, we modulate the frequency of the driven ac magnetic flux as . In the rotating frame, the interaction Hamiltonian reduces to


where and .

However, in the presence of , the frequencies of the delocalized cavity field modes and will be renormalized from the bare cavity frequency as and , respectively. Then, in the interaction picture, the field mode operators will be renormalized as


Therefore, the total interaction Hamiltonian reads


where and Assuming that , the above interaction can be treated as if it has two independent interaction channels that oscillate with distinctly different frequencies, with the cross talk between them being suppressed by a frequency difference of . When , the cross talk can be safely neglected. The effective Hamiltonian of the total interaction is


where and the Stark shift term has been neglected. In order to turn off this coupling td1 (); td2 (); td3 (); td4 (), we may modulate the coupling strength to be time dependent as , as recently demonstrated experimentally ccexp1 (); ccexp2 (), and the two cavities have a frequency difference of , with and being the resonant frequencies of the first and second cavities, respectively.

In subspace , the Hamiltonian in Eq. (21) becomes


where and the effective Rabi frequency . The effective Hamiltonian in Eq. (22) can be divided into two commuting parts as , with

When , the evolution operator in our logical qubit subspace reduces to

We can see that the gate in subspace is different from the one in subspace . Therefore, in general, this is a nontrivial two-qubit gate.

Figure 3: (Color online) Qubit-state population and fidelity dynamics of the gate as a function of dimensionless time .

For example, when and , it reduces to


In this case , which leads to , , , and thus MHz. In addition, and for . Moreover, the smallest oscillating frequency is when , and thus, the coupling between two transmons induced by the term is much smaller in strength compared with that induced by the term. Therefore, the higher-order terms are neglected in Eq. (18). For the initial state , we simulated the performance of this gate using the master equation with the total Hamiltonian in Eqs. (16), (17), and (18), as shown in Fig. 3, where a high fidelity of can be reached with the decay rates being the same as in the single-qubit case. The infidelity mainly comes from both the decoherence of the system and the validity of the effective Hamiltonian in Eq. (21), which are 3% and 2.5%, respectively. Meanwhile, considering the influence of the third level will additional introduce about 0.5% infidelity. In addition, when the anharmonicity is smaller, e.g., MHZ, the two-qubit fidelity will be 93.1% with MHz. Finally, as transmon 3 has a different frequency than the others, its coupling should not be the same as the others. This problem can be solved by redefining .

V Conclusion

In conclusion, we have proposed to implement HQC in DFS with the typical circuit QED, in which only two levels from conventional transmon qubits are required.

This work was supported by the NFRPC (Grants No. 2013CB921804 and No. 2011CB922104), the PCSIRT (Grant No. IRT1243), and the fund from NJU (Grant No. M28015).


  • (1) M. V. Berry, Proc. R. Soc. London Ser. A 392, 45 (1984).
  • (2) F. Wilczek, and A. Zee, Phys. Rev. Lett. 52, 2111 (1984).
  • (3) G. Falci, R. Fazio, G. M. Palma, J. Siewert, and V. Vedral, Nature (London) 407, 355 (2000).
  • (4) D. Leibfried, B. DeMarco, V. Meyer, D. Lucas, M. Barrett, J. Britton, W. M. Itano, B. Jelenković, C. Langer, T. Rosenband, and D. J. Wineland, Nature (London) 422, 412 (2003).
  • (5) J. Du, P. Zou, and Z. D. Wang, Phys. Rev. A 74, 020302(R) (2006).
  • (6) P. J. Leek, J. M. Fink, A. Blais, R. Bianchetti, M. Goppl, J. M. Gambetta, D. I. Schuster, L. Frunzio, R. J. Schoelkopf, and A. Wallraff, Science 318, 1889 (2007).
  • (7) M. Möttönen, J. J. Vartiainen, and J. P. Pekola, Phys. Rev. Lett. 100, 177201 (2008).
  • (8) M. Pechal, S. Berger, A.A. Abdumalikov, Jr., J. M. Fink, J. A. Mlynek, L. Steffen, A. Wallraff, and S. Filipp, Phys. Rev. Lett. 108, 170401 (2012).
  • (9) S.-L. Zhu and P. Zanardi, Phys. Rev. A 72, 020301(R) (2005).
  • (10) M. Johansson, E. Sjöqvist, L. M. Andersson, M. Ericsson, B. Hessmo, K. Singh, and D. M. Tong, Phys. Rev. A 86, 062322 (2012).
  • (11) P. Zanardi and M. Rasetti, Phys. Lett. A 264, 94 (1999).
  • (12) J. Pachos, P. Zanardi, and M. Rasetti, Phys. Rev. A 61, 010305(R) (1999).
  • (13) J. A. Jones, V. Vedral, A. Ekert, and G. Castagnoli, Nature (London) 403, 869 (2000).
  • (14) L.-M. Duan, J. I. Cirac, and P. Zoller, Science 292, 1695 (2001).
  • (15) A. Recati, T. Calarco, P. Zanardi, J. I. Cirac, and P. Zoller, Phys. Rev. A 66, 032309 (2002).
  • (16) L. Faoro, J. Siewert, and R. Fazio, Phys. Rev. Lett. 90, 028301 (2003).
  • (17) P. Zhang, Z. D. Wang, J. D. Sun, and C. P. Sun, Phys. Rev. A 71, 042301 (2005).
  • (18) O. Oreshkov, T. A. Brun, and D. A. Lidar, Phys. Rev. Lett. 102, 070502 (2009).
  • (19) V. N. Golovach, M. Borhani, and D. Loss, Phys. Rev. A 81, 022315 (2010).
  • (20) I. Kamleitner, P. Solinas, C. Müller, A. Shnirman, and M. Möttönen, Phys. Rev. B 83, 214518 (2011).
  • (21) N. Chancellor and S. Haas, Phys. Rev. A 87, 042321 (2013).
  • (22) K. Toyoda, K. Uchida, A. Noguchi, S. Haze, and S. Urabe, Phys. Rev. A 87, 052307 (2013).
  • (23) V. V. Albert, S. Krastanov, C. Shen, R.-B. Liu, R. J. Schoelkopf, M. Mirrahimi, M. H. Devoret, and L. Jiang, arXiv: 1503.00194.
  • (24) Wang Xiang-Bin and M. Keiji, Phys. Rev. Lett. 87, 097901 (2001).
  • (25) S. L. Zhu and Z. D. Wang, Phys. Rev. Lett. 89, 097902 (2002).
  • (26) E. Sjöqvist, D. M. Tong, L. M. Andersson, B. Hessmo, M. Johansson, and K. Singh, New J. Phys. 14, 103035 (2012).
  • (27) G. Feng, G. Xu, and G. Long, Phys. Rev. Lett. 110, 190501 (2013).
  • (28) A. A. Abdumalikov, Jr., J. M. Fink, K. Juliusson, M. Pechal, S. Berger, A. Wallraff, and S. Filipp, Nature (London) 496, 482 (2013).
  • (29) C. Zu, W.-B. Wang, L. He, W.-G. Zhang, C.-Y. Dai, F. Wang, and L.-M. Duan, Nature (London) 514, 72 (2014).
  • (30) S. Arroyo-Camejo, A. Lazariev, S. W. Hell, and G. Balasubramanian, Nat. Commun. 5, 4870 (2014).
  • (31) J. Koch, T. M. Yu, J. Gambetta, A. A. Houck, D. I. Schuster, J. Majer, A. Blais, M. H. Devoret, S. M. Girvin, and R. J. Schoelkopf, Phys. Rev. A 76, 042319 (2007).
  • (32) M. J. Peterer, S. J. Bader, X. Jin, F. Yan, A. Kamal, T. J. Gudmundsen, P. J. Leek, T. P. Orlando, W. D. Oliver, and S. Gustavsson, Phys. Rev. Lett. 114, 010501 (2015).
  • (33) L.-M. Duan, G.-C. Guo, Phys. Rev. Lett. 79, 1953 (1997).
  • (34) P. Zanardi, M. Rasetti, Phys. Rev. Lett. 79, 3306 (1997).
  • (35) D. A. Lidar, I. L. Chuang, K. B. Whaley, Phys. Rev. Lett. 81, 2594 (1998).
  • (36) L. A. Wu, P. Zanardi, and D. A. Lidar, Phys. Rev. Lett. 95, 130501 (2005).
  • (37) G. F. Xu, J. Zhang, D. M. Tong, E. Sjöqvist, and L. C. Kwek, Phys. Rev. Lett. 109, 170501 (2012).
  • (38) J. Zhang, L.-C. Kwek, E. Sjöqvist, D. M. Tong, and P. Zanardi, Phys. Rev. A 89, 042302 (2014).
  • (39) Z.-T. Liang, Y.-X. Du, W. Huang, Z.-Y. Xue, and H. Yan, Phys. Rev. A 89, 062312 (2014).
  • (40) G. Xu, G. Long, Sci. Rep. 4, 6814 (2014).
  • (41) J. Zhou, W.-C. Yu, Y.-M. Gao, and Z.-Y. Xue, Opt. Express 89, 14027 (2015).
  • (42) X. L. Feng, C. F. Wu, H. Sun, and C. H. Oh, Phys. Rev. Lett. 103, 200501 (2009).
  • (43) M. H. Devoret and R. J. Schoelkopf, Science 339, 1169 (2013).
  • (44) J. D. Strand, M. Ware, F. Beaudoin, T. A. Ohki, B. R. Johnson, A. Blais, and B. L. T. Plourde, Phys. Rev. B 87, 220505(R) (2013).
  • (45) A. Megrant, C. Neill, R. Barends, B. Chiaro, Y. Chen, L. Feigl, J. Kelly, E. Lucero, M. Mariantoni, P. J. J. O¡¯Malley, D. Sank, A. Vainsencher, J. Wenner, T. C. White, Y. Yin, J. Zhao, C. J. Palmstrøm, J. M. Martinis, and A. N. Cleland, Appl. Phys. Lett. 100, 113510 (2012).
  • (46) R. Barends, J. Kelly, A. Megrant, D. Sank, E. Jeffrey, Y. Chen, Y. Yin, B. Chiaro, J. Mutus, C. Neill, P. O’Malley, P. Roushan, J. Wenner, T. C. White, A. N. Cleland, and J. M. Martinis, Phys. Rev. Lett. 111, 080502 (2013).
  • (47) M. J. Hartmann, F. G. S. L. Brandão, and M. B. Plenio, Laser Photonics Rev. 2, 527 (2008).
  • (48) C. D. Ogden, E. K. Irish, and M. S. Kim, Phys. Rev. A 78, 063805 (2008).
  • (49) J. Bourassa, F. Beaudoin, J. M. Gambetta, and A. Blais, Phys. Rev. A 86, 013814 (2012).
  • (50) B. Peropadre, D. Zueco, F. Wulschner, F. Deppe, A. Marx, R. Gross, and J. J. García-Ripoll, Phys. Rev. B. 87, 134504 (2013).
  • (51) S. Felicetti, M. Sanz, L. Lamata, G. Romero, G. Johansson, P. Delsing, and E. Solano, Phys. Rev. Lett. 113, 093602 (2014).
  • (52) E. A. Sete, E. Mlinar, and A. N. Korotkov, Phys. Rev. B 91, 144509 (2015).
  • (53) Y. Yin, Y. Chen, D. Sank, P. J. J. O¡¯Malley, T. C. White, R. Barends, J. Kelly, E. Lucero, M. Mariantoni, A. Megrant, C. Neill, A.Vainsencher, J.Wenner, A. N.Korotkov, A. N. Cleland, and J. M. Martinis, Phys. Rev. Lett. 110, 107001 (2013).
  • (54) J. Wenner, Y. Yin, Y. Chen, R. Barends, B. Chiaro, E. Jeffrey, J. Kelly, A. Megrant, J. Y. Mutus, C. Neill, P. J. J. O¡¯Malley, P. Roushan, D. Sank, A. Vainsencher, T. C. White, A. N. Korotkov, A. N. Cleland, and J. M. Martinis, Phys. Rev. Lett. 112, 210501 (2014).
Comments 0
Request Comment
You are adding the first comment!
How to quickly get a good reply:
  • Give credit where it’s due by listing out the positive aspects of a paper before getting into which changes should be made.
  • Be specific in your critique, and provide supporting evidence with appropriate references to substantiate general statements.
  • Your comment should inspire ideas to flow and help the author improves the paper.

The better we are at sharing our knowledge with each other, the faster we move forward.
The feedback must be of minimum 40 characters and the title a minimum of 5 characters
Add comment
Loading ...
This is a comment super asjknd jkasnjk adsnkj
The feedback must be of minumum 40 characters
The feedback must be of minumum 40 characters

You are asking your first question!
How to quickly get a good answer:
  • Keep your question short and to the point
  • Check for grammar or spelling errors.
  • Phrase it like a question
Test description