Abstract
A quantum system interacts with its environment—if ever so slightly—no matter how much care is put into isolating it^{1}. Therefore, quantum bits undergo errors, putting dauntingly difficult constraints on the hardware suitable for quantum computation^{2}. New strategies are emerging to circumvent this problem by encoding a quantum bit nonlocally across the phase space of a physical system. Because most sources of decoherence result from local fluctuations, the foundational promise is to exponentially suppress errors by increasing a measure of this nonlocality^{3,4}. Prominent examples are topological quantum bits, which delocalize information over real space and where spatial extent measures nonlocality. Here, we encode a quantum bit in the field quadrature space of a superconducting resonator endowed with a special mechanism that dissipates photons in pairs^{5,6}. This process pins down two computational states to separate locations in phase space. By increasing this separation, we measure an exponential decrease of the bitflip rate while only linearly increasing the phaseflip rate^{7}. Because bitflips are autonomously corrected, only phaseflips remain to be corrected via a onedimensional quantum error correction code. This exponential scaling demonstrates that resonators with nonlinear dissipation are promising building blocks for quantum computation with drastically reduced hardware overhead^{8}.
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Data availability
The data that support the plots within this paper and other findings of this study are available from the corresponding author upon reasonable request.
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Acknowledgements
We acknowledge fruitful discussions with P. Rouchon and C. Smith. Z.L. acknowledges support from ANR project ENDURANCE and EMERGENCES grant ENDURANCE of Ville de Paris. A.S. acknowledges support from ANR project HAMROQS. The devices were fabricated within the consortium Salle Blanche Paris Centre. This work has been supported by the Paris ÎledeFrance Region in the framework of DIM SIRTEQ. M.M. acknowledges support from ARO under grant no. W911NF1810212. Z.L. acknowledges MinesParisTech as his primary affiliation.
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R.L. designed, fabricated and measured the device, and analysed the data. R.L. and Z.L. conceived the ATS element with help from B.H. and T.P. R.L. and Z.L. wrote the paper with input from all authors. M.V. fabricated the parametric amplifier. T.K. and M.D. provided experimental support. A.S. and M.M. provided theory support. Z.L. managed the project. All authors contributed to extensive discussions of the results.
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Peer review information Nature Physics thanks Christopher Eichler and the other, anonymous, reviewer(s) for their contribution to the peer review of this work.
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Extended data
Extended Data Fig. 1 Measured system parameters at the ATS working point.
The pump shifts the catqubit resonator and buffer frequencies. The frequencies in the absence of the pump are noted ω_{a∕b,0} and those in its presence are denoted ω_{a∕b}. The Kerr couplings χ_{mn} enter the full Hamiltonian in the form − χ_{mn}m^{†}mn^{†}n when m ≠ n and \(\frac{{\chi }_{mm}}{2}{{m}^{\dagger }}^{2}{m}^{2}\), where m, n denote the mode indices.
Extended Data Fig. 2 Underlying parameters of the catqubit and buffer resonators.
Measured and estimated circuit parameters (left), and their corresponding dipole energies (right).
Extended Data Fig. 3 Full device layout.
a, False color optical image of the ATS. Note that the 5 junction symbols are separated for clarity, the actual junctions are much closer and centered in the middle of the arm. b, False color optical image of the buffer. The buffer (red) is strongly coupled to its transmission line via an interdigitated capacitor (top). It is also capacitively coupled to the catqubit resonator (blue). This is actually a picture of a twin sample where this coupling was smaller. In panel c, the real size of the coupling capacitor is shown. (c) Full device layout. The catqubit resonator is coupled on its other side to a transmon qubit, itself coupled to a readout resonator which together enable to perform the catqubit tomography. After the interdigitated capacitor, the buffer input is filtered via three λ∕4stub filters. These stopband filters are centered at the catqubit resonance frequency to mitigate its direct coupling to the input line of the buffer^{44} (b). The onchip hybrid along the pump path (purple), equally splits the pump tone to RFflux bias the ATS with the right symmetry. The black lines linking two dots are a schematic representation of the crucial wirebonds of the device. The wirebonds linking the pump input to the onchip hybrid where implemented to reduce the area of the loop delimited by the center conductor and the ground plane, leading to a reduced sensitivity to flux noise.
Extended Data Fig. 4 RF and DC wiring of the dilution refrigerator.
Note that the pump and drive tones are attenuated at the base plate via directional couplers so that the attenuated power is dissipated at higher fridge stages, far from the sample. The I_{Σ} DC current and the RF pump signal are combined at 20 mK with a biastee. We have used a homemade ‘Snail Parametric Amplifier’ (SPA)^{45}.
Extended Data Fig. 5 Flux dependence.
a, Buffer spectroscopy. Phase of the reflected probe signal (colormap) on the buffer port as a function of \({I}_{_{\Sigma }}\) (xaxis) and probe frequency (yaxis). The buffer frequency follows an archlike pattern typical of SQUIDbased devices. The probing frequency range is limited to 38 GHz due to the 48 GHz circulator on the output line. The black dashed line represents the expected buffer/catqubit frequency for the best fitting parameter set. The slight aperiodicity may be explained by small asymmetries in the loop areas of the ATS. b, Catqubit resonator twotone spectroscopy. A continuous probe is applied on the catqubit resonator at various frequencies (yaxis) and a second tone attempts to πpulse the qubit on resonance. When the probe populates the catqubit, the qubit shifts in frequency due to the crossKerr coupling, and is insensitive to the πpulse. The resulting qubit occupation is plotted in color and we repeat the experiment for various values of \({I}_{_{\Sigma }}\) (xaxis). The black dashed line represents the expected buffer/catqubit frequency for the best fitting parameter set. The black vertical line corresponds to a flux bias were the buffer is at the qubit frequency resulting in a strong decrease in the qubit lifetime. c, For each value of \({I}_{_{\Sigma }}\) (xaxis) and \({I}_{_{\Delta }}\) (yaxis), we extract the buffer frequency from a spectroscopy measurement (panel a) and report it in color (white is when the resonance frequency is beyond the measurement range). Contrary to what they were designed for, the two flux lines do not perfectly apply symmetric (\({I}_{_{\Sigma }}\)) and antisymmetric (\({I}_{_{\Delta }}\)) bias on the ATS. We compensate for this imbalance while taking the data by shifting the \({I}_{_{\Sigma }}\) span for each value of \({I}_{_{\Delta }}\) as indicated on the xaxis label. Data were only taken on the area outside the hatched regions to prevent the heating of the dilution refrigerator beyond a tolerable temperature. The grey dashedrectangle corresponds to the flux range presented in Fig. 2 of the main text. d, Simulated flux dependence of the buffer mode for the best fitting parameter set.
Extended Data Fig. 6 Tuning the pump and drive frequencies.
a, Reflected relative drive amplitude (VNA measurement) as a function of drive frequency (xaxis) and pump frequency (yaxis). When ω_{p} = 2ω_{a} − ω_{d}, a sharp feature indicates that the twotoone photon exchange is resonant and as expected, it has a slope − 1. To observe this feature, we switch to the basis Δ = (Δ_{pump} + Δ_{drive})∕2, Δ_{b} = (Δ_{pump} − Δ_{drive})∕2, the orientation of which is given by the white dashed lines. b,c, Reflected relative drive amplitude (color) and parity of the catqubit resonator (red) as a function of Δ (xaxis) and Δ_{b} (yaxis) for increasing drive amplitude (top to bottom). The drive amplitude is expressed in units of the cat size ∣α_{∞}∣^{2} which is calibrated using the data of Extended Data Fig. 7. (c) When the twotoone photon exchange is resonant, the catqubit resonator is displaced and the parity drops to 0 if we measure after a time greater than \({\kappa }_{a}^{1}\). We also perform the catqubit resonator tomography and verify that the resonator is in a balanced mixture of \({\left0\right\rangle }_{\alpha }\) and \({\left1\right\rangle }_{\alpha }\). In all these plots, the white circles correspond to the chosen pump and drive frequencies. We verify that for all used drive amplitudes, this point remains centered in the resonant range. Therefore, we do not need to adapt the drive and pump frequencies when increasing the cat size. d, Cut of the color plot (c) at Δ_{b} = 0 representing the parity (open circle) of the catqubit steady state as a function of Δ. The relation of Eq. (26) of the supplementary information shows that the frequency window over which a nontrivial state is stabilized in the cavity scales as 2κ_{2}∣α∣^{2}. This enables us to determine κ_{2} assuming photon loss is the main loss mechanism. We fit (solid line) the measured parity with the expected steadystate parity (QuTiP) where the two fitting parameters are the parity contrast and κ_{2}. We find κ_{2}∕2π = 40 kHz.
Extended Data Fig. 7 Increasing the catqubit size.
a, Measured Wigner distribution of the catqubit state as a function of drive amplitude (left to right, top to bottom) after a pump and drive pulse duration of 20μs. b, Fitted cat size ∣α_{∞}∣^{2} (open circles) as a function of the drive amplitude ϵ_{d}. The drive amplitude is expressed in terms of the square root of the photon number the buffer would contain without the conversion process. For each Wigner distribution of panel (a), we fit a sum of two 2DGaussian functions (coherent states) diametrically opposed which are separated by a distance 2∣α_{∞}∣. Note that for simplicity, in the main text, we use ∣α∣^{2} instead of ∣α_{∞}∣^{2}. In the presence of single photon loss at rate κ_{a}, we expect ∣α_{∞}∣^{2} to follow the relation of Eq. (20) of the supplementary information (dashed line): a linear dependence on ϵ_{d} when α^{2} > κ_{a}∕(2κ_{2}). By fitting this relation to the data, we calibrate the xaxis scaling.
Extended Data Fig. 8 Equivalent circuit diagram.
The catqubit resonator (blue) is represented by a linear LC resonator with charging energy E_{C,a} and inductive energy E_{L,a}. It is capacitively coupled through a capacitor of charging energy E_{C,c} to the buffer (red) which consists of a capacitively shunted ATS element. The ATS, introduced in the main text, is formed by two Josephson junctions (crosses) of Josephson energies E_{J,1} and E_{J,2} split by an inductor of inductive energy E_{L,b}. In practice, this inductor is made out of 5 large Josephson junctions. Flux lines represented as grey inductors thread magnetic flux through the two ATS loops. One recovers the circuit of Fig. 2 by setting φ_{ext,1} = π and φ_{ext,2} = 0. Not shown here: the buffer is capacitively coupled to a transmission line and the catqubit resonator is coupled to a transmon qubit, its readout resonator and a transmission line.
Supplementary information
Supplementary Information
Supplementary Figs. 1–4 and Discussion.
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Lescanne, R., Villiers, M., Peronnin, T. et al. Exponential suppression of bitflips in a qubit encoded in an oscillator. Nat. Phys. 16, 509–513 (2020). https://doi.org/10.1038/s415670200824x
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