Abstract
Faulttolerant quantum computing relies on the ability to detect and correct errors, which in quantum error correction codes is typically achieved by projectively measuring multiqubit parity operators and by conditioning operations on the observed error syndromes. Here, we experimentally demonstrate the use of an ancillary qubit to repeatedly measure the ZZ and XX parity operators of two data qubits and to thereby project their joint state into the respective parity subspaces. By applying feedback operations conditioned on the outcomes of individual parity measurements, we demonstrate the realtime stabilization of a Bell state with a fidelity of Fâââ74% in up to 12 cycles of the feedback loop. We also perform the protocol using Pauli frame updating and, in contrast to the case of realtime stabilization, observe a steady decrease in fidelity from cycle to cycle. The ability to stabilize parity over multiple feedback rounds with no further reduction in fidelity provides strong evidence for the feasibility of executing stabilizer codes on timescales much longer than the intrinsic coherence times of the constituent qubits.
Introduction
The inevitable interaction of quantum mechanical systems with their environment renders quantum information vulnerable to decoherence.^{1,2,3} Quantum error correction aims to overcome this challenge by redundantly encoding logical quantum states into a largerdimensional Hilbert space and performing repeated measurements to detect and correct for errors.^{4,5,6,7} For sufficiently small error probabilities of individual operations, logical errors are expected to become increasingly unlikely when scaling up the number of physical qubits per logical qubit.^{8,9} As the concept of quantum error correction provides a clear path toward fault tolerant quantum computing,^{10} it has been explored in a variety of physical systems ranging from nuclear magnetic resonance,^{11} to trapped ions^{12,13,14,15} and superconducting circuits, both for conventional^{16,17,18,19} and for continuous variablebased encoding schemes.^{20}
Quantum error correction typically relies on the measurement of a set of commuting multiqubit parity operators, which ideally project the state of the data qubits onto a subspace of their Hilbert spaceâknown as the code spaceâwithout extracting information about the logical qubit state.^{7} A change in the outcome of repeated parity measurements signals the occurrence of an error, which brings the state of the qubits out of the code space. Such errors can either be corrected for in realtime by applying conditional feedback, or by keeping track of the measurement outcomes in a classical register to reconstruct the quantumstate evolution in post processing. The latter approachâalso known as Pauli frame updating^{21}âhas the advantage of avoiding errors introduced by imperfect feedback and additional decoherence due to feedback latency. Realtime feedback, on the other hand, could be beneficial in the presence of asymmetric relaxation errors, by preferentially mapping the qubits onto low energy states, which are more robust against decay.^{22} There are also important instances in which knowledge of the measurement results is required in real time to correctly choose subsequent operations, e.g., for the realization of logical nonClifford gates,^{7} for measurementbased quantum computing,^{23,24} and for stabilizing quantum states in cavity systems.^{20,25} Therefore, parity measurements, conditional feedback, and Pauli frame updating are all important elements for faulttolerant quantum computing, and are explored very actively.
Parity detection has previously been studied with superconducting circuits both with and without the use of ancillary qubits. Joint dispersive readout^{26,27} and the quantum interference of microwave signals^{28,29} were used to deterministically generate Bell states, and their stabilization was achieved by autonomous feedback based on reservoir engineering.^{17} Moreover, a recent theoretical proposal presented a protocol for direct weight4 parity detection.^{30} However, the most common approach for parity detection uses an ancillary qubit onto which the parity of the data qubits is mapped, and then projectively measured by reading out the ancillary state.^{31} By using two ancillary qubits, the simultaneous measurement of the XX and ZZ parity operators of two data qubits was demonstrated.^{32} Furthermore, ancillabased parity detection has enabled the realization of a threequbit bit flip code,^{18} a fivequbit repetition code,^{19} and the measurement of multiqubit parity operators for three^{33} and four^{34} data qubits. Repeated parity detection was also achieved using joint dispersive readout^{35} and for the cat code.^{36}
In most previous implementations of ancillabased parity detection, changes in the measured parity were accounted for in post processing rather than actively compensated for using feedback. Conditional feedback, however, was previously used in superconducting circuits to initialize and reset qubit states,^{37,38} to demonstrate a deterministic quantum teleportation protocol,^{39} to create and stabilize entanglement conditioned on a joint dispersive readout,^{27,35} and to extend the lifetime of a qubitstate encoded as a cat state in a superconducting cavity.^{20}
Here, we report on the experimental realization of repeated ancillabased XX and ZZ parity detection of two superconducting qubits. We perform realtime conditional feedback to stabilize the data qubits in a Bell state and to actively reset the ancillary qubit to the ground state, see Fig. 1. Our results are, thus, closely related to the recent experiments realized in a trapped ion system.^{40} We note that similar experiments using Pauli frame updating rather than realtime feedback have been performed in parallel with our work.^{41}
Results
The objective of the protocol is to stabilize two data qubits D1 and D2 in a target Bell state, chosen to be \(\Phi ^ + \rangle = (00\rangle + 11\rangle )/\sqrt 2\), for which both the XX and the ZZ parity are even, i.e., take the value +1, see Fig. 1a. We initially prepare both data qubits in an equal superposition state by applying a rotation \(R_y^\theta\) to both qubits with an angle Î¸â=âĎ/2 around the yaxis. We then map the parity of the joint state of D1 and D2 onto the ancillary qubit A by applying two controlled NOT gatesâdecomposed into conditional phase gates^{42} and singlequbit rotationsâwith the ancillary qubit as the target controlled by each of the data qubits. The subsequent measurement of A probabilistically yields the measurement result 0ă (1ă) for the ancilla qubit state, indicating the parity operator eigenvalue +1 (â1) and, ideally, projecting the joint state of D1 and D2 into the corresponding even (odd) parity subspace spanned by the basis states 00ă and 11ă (01ă and 10ă). The probability for each outcome depends on the input state, and is ideally 50% when initializing both qubits in an equal superposition state. After the measurement of A, we map the state of the data qubits into the even parity subspace by flipping the state of D2 with a \(R_x^\pi\) pulse if the parity measurement yields â1.^{37} In this case, we also reset the ancillary qubit to the ground state in preparation for the next round of parity detection.
Similarly, we perform XX parity measurements by changing the basis of D1 and D2 before and after the parity stabilization sequence with \(R_y^{ \pm \pi /2}\)pulses, see Fig. 1b. By choosing a feedback protocol that stabilizes both the XX and the ZZ parity to be even, we project the two data qubits onto the unique Bell state \(\Phi ^ + \rangle = (00\rangle + 11\rangle )/\sqrt 2\) in two subsequent rounds of parity feedback. Repeating these two parity stabilization steps sequentially ideally stabilizes this Bell state indefinitely. The main requirements for the realization of this protocol are (i) high fidelity and fast readout of the ancillary qubit with little disturbance of the data qubits, (ii) high fidelity single and twoqubit gates, (iii) low latency classical electronics to perform conditional feedback with delay times much shorter than the qubit coherence times, and (iv) the absence of leakage into noncomputational states.
We implement this parity stabilization protocol on a small superconducting quantum processor consisting of a linear array of four transmon qubits, of which each pair of nearest neighbors is coupled via a detuned resonator,^{43} see Fig. 2. Each qubit has individual charge (pink) and flux control lines (green) to perform singlequbit gates and to tune the qubit transition frequency. Each of the four qubits is coupled to an individual readout circuit used for probing the state of the qubits by frequency multiplexed dispersive readout through a common feedline (purple).^{44} Further details of the device and its fabrication are discussed in the Methods section. We mount this fourqubit device at the base plate of a cryogenic measurement setup, equipped with input and output lines, specified in Supplementary Note 2, for microwave control and detection.
For our experiments, we use the three qubits labeled D1, A, and D2 in Fig. 2. We perform singlequbit gates in 50âns using DRAG pulses^{45} with an average gate error of 0.3% characterized by randomized benchmarking.^{46} The average error remains below 0.38% for all qubits when characterized by simultaneous randomized benchmarking,^{47} which indicates small crosstalk of the singlequbit gates. Singlequbit gate fidelities are mostly limited by the coherence times, which range from 14 to 23âÎźs (15 to 22âÎźs) for T_{1} (\(T_2^{\mathrm{E}}\)), see Supplementary Table 1. Conditional phase gates are realized with flux pulses on the data qubits in ~180âns, by tuning the 11ă state into resonance with the 20ă state for a full period of the resonant exchange interaction,^{42} see also Supplementary Note 2. By calibrating and correcting for flux pulse distortion, we achieve twoqubit gate fidelities of 98.8% (99.4%) for the gate between D1 and A (D2 and A) characterized using quantum process tomography,^{48} while the gate fidelity limit due to decoherence is calculated to be 99.2% (99.5%). The dynamical phases acquired during the flux pulses are compensated using virtualZ gates.^{49} Using a readout pulse length of 200âns and an integration time of 400âns, see the Methods section, we achieve an average probability for correct readout assignment close to 99% when reading out all three qubits simultaneously.
We characterize the coherent part of the parity detection algorithm by performing quantumstate tomography of all three qubits prior to the first readout of A. Accounting for finite readout fidelity, we average this data to obtain the expectation values for all multiqubit Pauli operators \(\hat P\) (Fig. 3a). The overall threequbit state fidelity Fâ=âăĎĎĎăâââ94%, estimated based on the most likely density matrix Ď reconstructed from the measured Pauli sets, is in good agreement with the fidelity of 92.8%, calculated using a master equation simulation accounting for qubit decoherence and residual ZZ coupling (for details, see Supplementary Note 3). The finite XY correlations, which are well reproduced by the numerical simulations, are due to the residual ZZ coupling between the data qubits and the ancillary qubit with rates 110 and 370âkHz for D1 and D2, respectively, which we do not compensate for during the coherent part of the protocol. A reduction of residual ZZ coupling could, e.g., be achieved with alternative coupling schemes featuring larger onâoff ratios.^{50,51,52}
In a next step, we characterize the state of D1 and D2 conditioned on the outcome of the first ancilla measurement using twoqubit state tomography, see Fig. 3b, c. In this experiment, both D1 and D2 are read out simultaneously with A. For both parity measurement outcomes +1 and â1, projecting D1 and D2 into the even and odd parity Bell state ÎŚ^{+}ă and Î¨^{+}ă, respectively, we find the resulting fidelities (93.8% and 92.9%) to be close to the ones obtained by projecting the reconstructed threequbit state onto the corresponding twoqubit subspaces (95.9% and 93.4%). This level of agreement is consistent with the high readout assignment probability of 98.7% of the ancillary qubit. Most importantly, we find the outcome of the ancilla measurement to correlate very well with the sign of the resulting ZZ correlations of the data qubits, indicating that the parity measurement is highly projective. More specifically, we find ăZZăâ=â+0.86 (â0.89) conditioned on having measured A in the ground (excited) state.
To prepare the specific target state \(\Phi ^ + \rangle = (00\rangle + 11\rangle )/\sqrt 2\) deterministically, we apply a Ďpulse to qubit D2 if the ancilla measurement yields an odd parity â1, compare circuit diagram in Fig. 1b. Alternatively, we could prepare the state \(\Psi ^ + \rangle = (10\rangle + 01\rangle )/\sqrt 2\), by changing the condition for feedback, i.e., applying the feedback pulse if the parity is even. The feedback scheme chosen here, maps the oddparity state characterized in Fig. 3c to the evenparity state in Fig. 3b. Indeed, the resulting unconditional state has a fidelity of 86.7% indicating that we correctly prepare the desired target state, see Fig. 3d. According to the comparison with master equation simulations (see Supplementary Note 3 for details), the reduced fidelity is dominated by qubit decoherence during the delay time of 1âÎźs between the parity detection and the application of the feedback pulse to D2. We partly mitigate the dephasing and the residual ZZ interaction by applying four dynamical decoupling pulses using the CarrâPurcellâMeiboomâGill (CPMG) protocol to the data qubits during the feedback delay time, see pulse sequence in Supplementary Note 2. We observe deterministic phase shifts of both data qubits after completion of the ancilla readout, which we attribute to a measurementinduced Stark shift due to the offresonant driving of coupling resonators by the ancilla readout pulse.^{53} We compensate for these phase shifts by inserting virtualZ gates after the ancilla readout. However, we possibly overcorrect this source of error and, thus, observe smaller phase errors (ăXYă and ăYXă) in the experiment than expected from simulations (Fig. 3d).
We emphasize that the XX and YY correlations, measured after the ZZ parity check (Fig. 3d), are a consequence of the specific initial state (00ăâ+â01ăâ+â10ăâ+â11ă)/2, which we prepare prior to mapping onto the even ZZ parity subspace. For the more general case of, e.g., a mixed initial state, we observe a nearly vanishing ăXXă correlation of 0.011 after mapping onto the even ZZ subspace, as expected. Creating and stabilizing finite XX [and YYâ=ââ(XX)(ZZ)] correlations, therefore requires a consecutive measurement of the commuting XX parity operator and the projection of D1 and D2 into the corresponding subspace. We achieve this by enclosing the ZZ parity stabilization pulse sequence in appropriately chosen basis change rotations, see Fig. 1b. The resulting state has a fidelity of 74.5% compared with the target state ÎŚ^{+}ă (Fig. 3e), close to the simulated value of 75.8%. From simulations, we find that the reduction in fidelity relative to the previous round of parity feedback is dominated by the additional dephasing of data qubits during the XX stabilization cycle.
Most importantly, we also demonstrate the repeatability of parity detection and stabilization which is a crucial requirement for quantum error correction. Specifically, we characterize the evolution of the prepared quantum state for up to 12 cycles of ZZ or XX parity stabilization sequences. We first repeatedly measure the ZZ parity and stabilize the state in the even ZZ subspace. In this case, we observe a decrease of the measured Bellstate fidelity to ~50% after Nâ=â12 cycles (green points in Fig. 4a). This experimental observation is in agreement with master equation simulations and due to the decoherence of the initial ăXXă correlations, which are not stabilized by the repeated ZZ parity checks, see green symbols in Fig. 4c. When the ZZ parity stabilization is paired with a subsequent XX parity stabilization, we observe the expected unconditional stabilization of the target Bell state. Already after a single pair of stabilization cycles (Nâ=â2), the Bellstate fidelity reaches a steadystate value of ~74%, which is maintained for all subsequent stabilization cycles. In agreement with simulations, the ăXXă correlations are now stabilized as well and they take higher values than ăZZă because we characterize the state only after stabilizing each even N rounds of feedback, i.e., after stabilizing XX.
To gain further insights into the feedback process, we also perform the experiment using Pauli frame updates (PFU) rather than applying feedback pulses to the data qubits while still using feedback for resetting the ancilla qubit. Here, we keep track of the parity measurements in software, and apply Pauli frame updating to stabilize the target subspaces. The gate sequence is then equivalent to Fig. 1, but feedback is only used for resetting the ancilla qubit after each parity measurement. As the ancilla is reset in every stabilization round, the Pauli frame update is only conditioned on the last two (one) parity measurements when stabilizing both ZZ and XX (only ZZ) as these two (one) measurements completely determine the corresponding Pauli frame. Thus, if the last ZZ (XX) outcome is â1, we apply a \(R_x^\pi\) (\(R_z^\pi\)) rotation to the Pauli operators of the state tomography of D2 before averaging the data and reconstructing the most likely density matrix.
In Fig. 4d, we observe that the initialstate fidelity is slightly above the one of the active stabilization protocol in Fig. 4a; however, the fidelity now decreases when repeating the protocol. In the end, we observe a 10% lower Bellstate fidelity after Nâ=â12 cycles, half of which is expected from simulations. We attribute the decrease in fidelity to the asymmetry of relaxation errors.^{22} When the data qubits are not actively stabilized in the even subspaces of the parity operators, the ancilla qubit ends up in the 1ăstate more often. Thus, during the feedback delay, there is a higher chance of T_{1}errors on the ancilla qubit, which will propagate into the next parity measurement cycle. We also expect that the residual ZZ errors, when the ancilla is in the excited state, lead to accumulated phase errors in ăXXă when only stabilizing ZZ, see Fig. 4f. These accumulated errors are observed in the data and are reproduced in the simulations. Beyond the errors predicted by the simulations, we observe an additional decay of the ăZZă correlations. While these errors are significantly larger than expected from simulations, they could be explained by additional measurementinduced transitions from the 1ăstate to the secondexcited state of the ancilla qubit during readout. A systematic characterization of leakage errors, caused by both measurementinduced mixing^{54} and twoqubit gates,^{55} could be an interesting topic for future investigations.^{41}
Discussion
In conclusion, we demonstrated the stabilization of a Bell state by repeated parity detection combined with conditional realtime feedback. More generally, our experiment demonstrates the use of projective stabilizer measurements to establish coherence between multiple qubits. The measurement acts selectively on the ancilla qubit avoiding measurementinduced dephasing of the data qubits by using individual Purcell filters. Our comparison with Pauli frame updating provides evidence for potential advantages of realtime feedback control for quantum error correction by avoiding errors due to relaxation of the ancilla qubits, a topic to be further investigated. From numerical simulations, by excluding decoherence from the simulation, we find that our protocol stabilizes the target state at 94.9% fidelity limited by readout errors and residual ZZ coupling. Thus, the measured steadystate fidelity is mainly limited by decoherence during the feedback delay time of 1âÎźs, which we expect to further decrease in the future by reducing the latency of feedback electronics^{38} and the readout duration.^{56,57,58,59} Our results constitute an important step toward the realtime stabilization of entangled multiqubit states beyond Bell states using higherweight parity detection^{33,34} as required, for example, in quantum error correction codes, such as the BaconShor code^{60} and the surface code.^{8,9}
Methods
Sample design and fabrication
The device in Fig. 2 of the main text consists of four qubits coupled to each other in a linear chain. All resonators, coupling capacitors, control lines, and qubit islands are fabricated from a 150ânm thin niobium film sputtered onto a highresistivity intrinsic silicon substrate, which is patterned using photolithography and reactive ion etching. We further add airbridges to the device to establish a wellconnected ground plane across the chip. The Josephson junctions of the qubits are fabricated using electronbeam lithography and shadow evaporation of aluminum. As shown in Fig. 5b, the junctions are arranged in a SQUID loop (blue) and contacted to the niobium film (gray and yellow) using an additional bandage of aluminum (red).^{61,62}
The qubits are connected via a readout resonator and a Purcell filter to a common feedline used for frequency multiplexed readout, see Fig. 5a and ref. ^{44} for details of this readout architecture. The capacitive coupling elements between the Purcell filters and the feedline, see Fig. 5c, are designed to have a larger minimal feature size of 6âÎźm, compared with the 3âÎźm of our standard interdigitated capacitors, making their capacitance, and thus the frequencies and linewidths of the Purcell filters, less sensitive to slight variations in the photolithography process. The qubits are designed to have a charging energy of 270âMHz set by the total capacitance of the qubit island. An asymmetric SQUID reduces their sensitivity to flux noise.^{63} From a fit to the measured qubit frequencies as a function of magnetic flux bias, we extract a SQUID asymmetry of ~1:8 for all three qubits. To achieve a large mutual inductance of Mâââ1.6âpH, we place the SQUID close to the shorted end of the flux line.
Qubitâqubit interactions are mediated by transmission line resonators, see Fig. 5d. Since the coupling strength J is proportional to the impedance of the coupling resonator,^{43,64} we increase the characteristic impedance for segments of the transmission line resonator to Z_{0}âââ80âÎŠ compared with the standard value of 50âÎŠ. We achieve this increase in impedance by increasing the separation between center conductor and ground plane, which results in a smaller capacitance per unit length. The center segment is kept at the standard value of 50âÎŠ to accommodate an airbridge crossing the resonator to connect the ground planes on both sides of the coupler. The resulting qubitâqubit exchange rate is measured to be J_{10â01}/2Ďâââ3.8(3.4)âMHz at the interaction point of the twoqubit gates between qubits D1 (D2) and A. In addition, we characterized the qubit parameters using standard spectroscopy and timedomain measurements, see Supplementary Note 1.
Readout characterization
With the dispersive shifts Ď and the resonator linewidths Îş_{eff} listed in Supplementary Table 1, we measure correct readout assignment probabilities of ~99%, for both individual and multiplexed readout, the agreement of which indicates low readout crosstalk.^{44} For this readout, we used a 200âns long, squareshaped readout pulse. Due to the finite response time of the readout resonator, the resulting output signal is ~400âns long. In order to maximize distinguishability between the states, we use a 400âns long modematched filter for integrating this signal.^{44} More specifically, we also characterize the multiqubitstate assignment and find a probability of more than 95% to correctly assign any threequbit state, see Fig. 6. We also extract the average crossmeasurementinduced dephasing rate, \({\bar{\mathrm \Gamma }}_{ij}\), from the loss of contrast in the Ramsey signal of qubit Qi when interleaving a readout pulse on qubit Qj between two Ramsey pulses.^{44,65} We find that the probability of inducing a phase error on the data qubits due to the ancilla readout pulse is <0.3%, see Fig. 7. We observe, however, that the readout of qubit A induces a deterministic phase shift on qubits D1 and D2 of 33.4Â° and 33.2Â°, respectively, which we attribute to measurementinduced Stark shifts from offresonantly driving the coupling resonators. In the parity stabilization protocol, we compensate for these phase shifts using virtualZ gates.^{49}
Data availability
The data produced in this work is available from the corresponding author upon reasonable request.
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Acknowledgements
The authors thank A. Blais, B. Royer, J. M. Renes, and J. Home for valuable feedback on the paper and J. Butscher, F. Bruckmaier, and M. Bild for contributions to the experimental setup and the control software. The authors acknowledge financial support by the Office of the Director of National Intelligence (ODNI), Intelligence Advanced Research Projects Activity (IARPA), via the U.S. Army Research Office grant W911NF1610071, by the National Centre of Competence in Research Quantum Science and Technology (NCCR QSIT), a research instrument of the Swiss National Science Foundation (SNSF), the EU Flagship on Quantum Technology H2020FETFLAG201803 project 820363 OpenSuperQ and by ETH Zurich. The views and conclusions contained herein are those of the authors, and should not be interpreted as necessarily representing the official policies or endorsements, either expressed or implied, of the ODNI, IARPA, or the U.S. Government.
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C.K.A., A.R., S.K., J.H., A.W. and C.E. designed the experiment. C.K.A. designed the device and A.R., S.K., J.C.B. and M.G. fabricated the device. C.K.A., A.R., S.L., S.K. and J.H. set up the experiment and wrote the experimental control software. C.K.A., A.R. and S.L. carried out the experiment, analyzed all data, and produced all figures. C.K.A. and S.L. performed the numerical simulations. A.W. and C.E. supervised the work. C.K.A., A.W. and C.E. wrote the paper with input from all coauthors.
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Andersen, C.K., Remm, A., Lazar, S. et al. Entanglement stabilization using ancillabased parity detection and realtime feedback in superconducting circuits. npj Quantum Inf 5, 69 (2019). https://doi.org/10.1038/s4153401901854
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DOI: https://doi.org/10.1038/s4153401901854
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