Skip to main content

Thank you for visiting nature.com. You are using a browser version with limited support for CSS. To obtain the best experience, we recommend you use a more up to date browser (or turn off compatibility mode in Internet Explorer). In the meantime, to ensure continued support, we are displaying the site without styles and JavaScript.

# A fast quantum interface between different spin qubit encodings

## Abstract

Single-spin qubits in semiconductor quantum dots hold promise for universal quantum computation with demonstrations of a high single-qubit gate fidelity above 99.9% and two-qubit gates in conjunction with a long coherence time. However, initialization and readout of a qubit is orders of magnitude slower than control, which is detrimental for implementing measurement-based protocols such as error-correcting codes. In contrast, a singlet-triplet qubit, encoded in a two-spin subspace, has the virtue of fast readout with high fidelity. Here, we present a hybrid system which benefits from the different advantages of these two distinct spin-qubit implementations. A quantum interface between the two codes is realized by electrically tunable inter-qubit exchange coupling. We demonstrate a controlled-phase gate that acts within 5.5 ns, much faster than the measured dephasing time of 211 ns. The presented hybrid architecture will be useful to settle remaining key problems with building scalable spin-based quantum computers.

## Introduction

Initialization, single-qubit and two-qubit gate operations, and measurements are fundamental elements for universal quantum computation1. Generally, they should all be fast and with high fidelity to reach the fault-tolerance thresholds2. So far, various encodings of spin qubits into one to three-spin subspaces have been developed in semiconductor quantum dots3,4,5,6,7,8,9,10,11,12,13,14,15. In particular, recent experiments demonstrated all of these elements including two-qubit logic gates for single-spin qubits proposed by Loss and DiVincenzo (LD qubits) and singlet-triplet (ST) qubits6,7,8,14. These qubits have different advantages depending on the gate operations, and combinations thereof can increase the performance of spin-based quantum computing. In LD qubits, the two-qubit gate is fast6,7 as it relies on the exchange interaction between neighboring spins. In contrast, the two-qubit gate in ST qubits is much slower as it is mediated by a weak dipole coupling14. Concerning initialization and readout, however, the situation is the opposite: it is slow for LD qubits, relying on spin-selective tunneling to a lead16,17, while it is orders of magnitude faster in ST qubits relying on Pauli spin blockade12,13. Therefore, a fast and reliable interface between LD and ST qubits would allow for merging the advantages of both realizations.

Here we present such an interface implementing a controlled-phase (CPHASE) gate between a LD qubit and a ST qubit in a quantum dot array18,19. The gate is based on the nearest neighbor exchange coupling and is performed in 5.5 ns. Even though we do not pursue benchmarking protocols here, the gate time being much shorter than the corresponding dephasing time (211 ns) indicates that the fidelity of this type of gates can be very high. Our results demonstrate that controlled coherent coupling of different types of gated spin qubits is feasible, and one can proceed to combining their advantages. Overall, our work pushes further the demonstrated scalability of spin qubits in quantum dot arrays.

## Results

### A LD qubit and a ST qubit formed in a triple quantum dot (TQD)

A hybrid system comprising a LD qubit and a ST qubit is implemented in a linearly-coupled gate-defined TQD shown in Fig. 1a. The LD qubit (QLD) is formed in the left dot while the ST qubit (QST) is hosted in the other two dots. We place a micro-magnet near the TQD to coherently and resonantly control QLD via electric dipole spin resonance (EDSR)20,21,22,23,26. At the same time it makes the Zeeman energy difference between the center and right dots, $${\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}}$$, much larger than their exchange coupling JST, such that the eigenstates of QST become |↑↓〉 and |↓↑〉 rather than singlet |S〉 and triplet |T〉. We apply an external in-plane magnetic field Bext = 3.166 T to split the QLD states by the Zeeman energy EZ as well as to separate polarized triplet states |↑↑〉 and |↓↓〉 from the QST computational states. The experiment is conducted in a dilution refrigerator with an electron temperature of approximately 120 mK. The qubits are manipulated in the (NL, NC, NR) = (1,1,1) charge state while the (1,0,1) and (1,0,2) charge states are also used for initialization and readout (see Fig. 1b). Here, NL(C,R) denotes the number of electrons inside the left (center, right) dot.

We first independently measure the coherent time evolution of each qubit to calibrate the initialization, control, and readout. We quench the inter-qubit exchange coupling by largely detuning the energies of the (1,1,1) and (2,0,1) charge states. For QLD, we observe Rabi oscillations4 with a frequency fRabi of up to 10 MHz (Fig. 1d) as a function of the microwave (MW) burst time tMW, using the pulse sequence in Fig. 1e. For QST, we observe the precession between |S〉 and |T〉 (ST precession) (Fig. 1f) as a function of the evolution time te, using the pulse sequence in Fig. 1g (see Supplementary Note 2 for full control of QST). We use a metastable state to measure QST with high fidelity13 (projecting to |S〉 or |T〉) in the presence of large $${\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}}$$ with which the lifetime of |T〉 is short27.

### Calibration of the two-qubit coupling

The two qubits are interfaced by exchange coupling JQQ between the left and center dots as illustrated in Fig. 1c. We operate the two-qubit system under the conditions of $$E_{\mathrm{Z}} \gg {\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}},{\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{QQ}}} \gg J^{{\mathrm{QQ}}} \gg J^{{\mathrm{ST}}}$$ where $${\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{QQ}}}$$ is the Zeeman energy difference between the left and center dots. Then, the Hamiltonian of the system is

$${\cal H} = - E_{\mathrm{Z}}\hat \sigma _z^{{\mathrm{LD}}}/2 - {\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}}\hat \sigma _z^{{\mathrm{ST}}}/2 + J^{{\mathrm{QQ}}}(\hat \sigma _z^{{\mathrm{LD}}}\hat \sigma _z^{{\mathrm{ST}}} - 1)/4$$
(1)

where $$\hat \sigma _z^{{\mathrm{LD}}}$$ and $$\hat \sigma _z^{{\mathrm{ST}}}$$ are the Pauli z-operators of QLD and QST, respectively18 (Supplementary Note 3). The last term in Eq. (1) reflects the effect of the inter-qubit coupling JQQ: for states in which the spins in the left and center dots are antiparallel, the energy decreases by JQQ/2 (see Fig. 2a). In the present work, we choose to operate QLD as a control qubit and QST as a target, although these are exchangeable. With this interpretation, the ST precession frequency fST depends on the state of QLD, $$f_{\sigma _z^{{\mathrm{LD}}}}^{{\mathrm{ST}}} = \left( {{\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}} - \sigma _z^{{\mathrm{LD}}}J^{{\mathrm{QQ}}}/2} \right)/h$$. Here $$\sigma _z^{{\mathrm{LD}}}$$ represents |↑〉 or |↓〉 and +1 or −1 interchangeably. This means that while JQQ is turned on for the interaction time tint, QST accumulates the controlled-phase ϕC = 2πJQQtint/h, which provides the CPHASE gate (up to single-qubit phase gates; see Supplementary Note 7) in tint = h/2JQQ. An important feature of this two-qubit gate is that it is intrinsically fast, scaling with JQQ/h which can be tuned up to ~100 MHz, and is limited only by the requirement $$J^{{\mathrm{QQ}}}/h \ll {\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{QQ}}}/h \sim 500\,{\mathrm{MHz}}$$ in our device.

Before testing the two-qubit gate operations, we calibrate the inter-qubit coupling strength JQQ, and its tunability by gate voltages. The inter-qubit coupling in pulse stage F (Fig. 2b) is controlled by the detuning energy between (2,0,1) and (1,1,1) charge states (one of the points denoted E in Fig. 1b). To prevent leakage from the QST computational states, we switch JQQ on and off adiabatically with respect to $${\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{QQ}}}$$ by inserting voltage ramps to stage F with a total ramp time of tramp = 24 ns (Fig. 2b)28. The coherent precession of QST is measured by repeating the pulse stages from D to H without initializing, controlling and measuring QLD, which makes QLD a random mixture of |↑〉 and |↓〉. Figure 2c shows the FFT spectra of the precession measured for various interaction points indicated in Fig. 1b. As we bring the interaction point closer to the boundary of (1,1,1) and (2,0,1), JQQ becomes larger and we start to see splitting of the spectral peaks into two. The separation of the two peaks is given by JQQ/h which can be controlled by the gate voltage as shown in Fig. 2d.

We now demonstrate the controllability of the ST precession frequency by the input state of QLD, the essence of a CPHASE gate. We use the quantum circuit shown in Fig. 2b, which combines the pulse sequences for independent characterization of QLD and QST. Here we choose the interaction point such that JQQ/h = 90 MHz. By using either |↑〉 or |↓〉 as the QLD initial state (the latter prepared by an EDSR π pulse), we observe the ST precessions as shown in Fig. 2e, f. The data fit well to Gaussian-decaying oscillations giving $$f_{| \uparrow \rangle}^{{\mathrm{ST}}} = 434 \pm 0.5\,{\mathrm{MHz}}$$ and $$f_{| \downarrow \rangle}^{{\mathrm{ST}}} = 524 \pm 0.4\,{\mathrm{MHz}}$$ [These are consistent with the values determined by Bayesian estimation discussed in Methods]. This demonstrates the control of the precession rate of QST by JQQ/h depending on the state of QLD.

### Demonstration of a CPHASE gate

To characterize the controlled-phase accumulated during the pulse stage F, we separate the phase of QST into controlled and single-qubit contributions as $$\phi _{\sigma _z^{{\mathrm{LD}}}} = - \pi \sigma _z^{{\mathrm{LD}}}J^{{\mathrm{QQ}}}\left( {t_{{\mathrm{int}}} + t_0} \right)/h$$ and $$\phi ^{{\mathrm{ST}}} = 2\pi {\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}}( {t_{{\mathrm{int}}} + t_{{\mathrm{ramp}}}} )/h + \phi _0$$, respectively. Here t(tramp) represents the effective time for switching on and off JQQ (Supplementary Note 5). A phase offset ϕ0 denotes the correction accounting for nonuniform $${\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}}$$ during the ramp (Supplementary Note 5). Then the probability of finding the final state of QST in singlet is modeled as

$$P_{{\mathrm{S}},{\mathrm{model}}} = a{\mathrm{cos}}\left( {\phi _{\sigma _z^{{\mathrm{LD}}}} + \phi ^{{\mathrm{ST}}}} \right)\exp \left( { - (t_{{\mathrm{int}}}/T_2^ \ast )} \right)^2 + b$$
(2)

where a, b and $$T_2^ \ast$$ represent the values of amplitude, mean and the dephasing time of the ST precession, respectively. We use maximum likelihood estimation (MLE) combined with Bayesian estimation29,30 to fit all variables in Eq. 2, that are $$a,b,t_0,J^{{\mathrm{QQ}}},T_2^ \ast ,\phi _0$$, and $${\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}}$$, from the data (Methods). This allows us to extract the tint dependence of $$\phi _{\sigma _z^{{\mathrm{LD}}}}$$ (Fig. 3a) (Methods) and consequently ϕC = ϕ|↓〉 − ϕ|↑〉 (Fig. 3b). It evolves with tint in the frequency of JQQ/h = 90 MHz, indicating that the CPHASE gate time can be as short as h/2JQQ = 5.5 ns (up to single-qubit phase). On the other hand, $$T_2^ \ast$$ obtained in the MLE is 211 ns, much longer than what is observed in Fig. 2e, f because the shorter data acquisition time used here cuts off the low-frequency component of the noise spectrum29. We note that this $$T_2^ \ast$$ is that for the two-qubit gate while JQQ is turned on8, and therefore it is likely to be dominated by charge noise rather than the nuclear field fluctuation (Supplementary Note 6). The ratio $$2J^{{\mathrm{QQ}}}T_2^ \ast /h$$ suggests that 38 CPHASE operations would be possible within the two-qubit dephasing time. We anticipate that this ratio can be further enhanced by adopting approaches used to reduce the sensitivity to charge noise in exchange gates such as symmetric operation31,32 and operation in an enhanced field gradient33.

Finally we show that the CPHASE gate operates correctly for arbitrary QLD input states. We implement the circuit shown in Fig. 4a in which tint is fixed to yield ϕC = π, while a coherent initial QLD state with an arbitrary $$\sigma _z^{{\mathrm{LD}}}$$ is prepared by EDSR. We extract the averaged $$\phi _{\sigma _z^{{\mathrm{LD}}}}$$, $$\left\langle \phi _{\sigma _z^{{\mathrm{LD}}}} \right\rangle$$ by Bayesian estimation29,30, which shows an oscillation as a function of tMW in agreement with the Rabi oscillation measured independently by reading out QLD at stage C as shown in Fig. 4b (see Methods for the estimation procedure and the origin of the low visibility, i.e., $${\mathrm{max}}| {\langle {\phi _{\sigma _z^{{\mathrm{LD}}}}} \rangle } | < \pi /2$$). These results clearly demonstrate the CPHASE gate functioning for an arbitrary QLD input state.

## Discussion

In summary, we have realized a fast quantum interface between a LD qubit and a ST qubit using a TQD. The CPHASE gate between these qubits is performed in 5.5 ns, much faster than its dephasing time of 211 ns and those ratio (~38) would be high enough to provide a high-fidelity CPHASE gate (Supplementary Note 8). Optimizing the magnet design to enhance the field gradient would allow even faster gate time beyond GHz with larger JQQ. At the same time, this technique is directly applicable to Si-based devices with much better single-qubit coherence5,6,7,8,9. Our results suggest that the performance of certain quantum computational tasks can be enhanced by adopting different kinds of qubits for different roles. For instance, LD qubits can be used for high-fidelity control and long memory and the ST qubit for fast initialization and readout. This combination is ideal for example, the surface code quantum error correction where a data qubit must maintain the coherence while a syndrome qubit must be measured quickly34. Furthermore, the fast (~100 ns25) ST qubit readout will allow the read out of a LD qubit in a quantum-non-demolition manner35 with a speed three orders of magnitude faster than a typical energy-selective tunneling measurement16,17. Viewed from the opposite side, we envisage coupling two ST qubits through an intermediate LD qubit, which would boost the two ST qubit gate speed by orders of magnitude compared to the demonstrated capacitive coupling scheme14. In addition, our results experimentally support the concept of the theoretical proposal of a fast two-qubit gate between two ST qubits based on direct exchange36 which shares the same working principle as our two-qubit gate. Our approach will further push the demonstrated scalability of spin qubits in quantum dot arrays beyond the conventional framework based on a unique spin-qubit encoding.

## Methods

### Device design

Our device was fabricated on a GaAs/Al0.3Ga0.7As heterostructure wafer having a two-dimensional electron gas 100 nm below the surface, grown by molecular beam epitaxy on a semi-insulating (100) GaAs substrate. The electron density n and mobility μ at a temperature of 4.2 K are n = 3.21 × 1015 m−2 and μ = 86.5 m2 V−1 s−1 in the dark, respectively. We deposited Ti/Au gate electrodes to define the TQD and the charge sensing single electron transistor. A piece of Co metal (micro-magnet, MM) is directly placed on the surface of the wafer to provide a local magnetic field gradient in addition to the external magnetic field applied in-plane (along z). The MM geometry is designed based on the numerical simulations of the local magnetic field23. The field property is essentially characterized by the two parameters23: dBx/dz at the position of each dot and the difference in Bz between the neighboring dots, ΔBz (see Fig. 1a for the definition of the x and z axes). dBx/dz determines the spin rotation speed by EDSR and is as large as ~1 mT nm−1 at the left dot (Supplementary Fig. 5a) allowing fast control of QLD (fRabi > 10 MHz)20,23. At the same time ΔBz between the left and center dots, $${\mathrm{\Delta }}B_z^{{\mathrm{LC}}}$$, is designed to be ~60 mT (Supplementary Fig. 5b) to guarantee the selective EDSR control of QLD without rotating the spin in the center dot20,23. Furthermore, ΔBz between the center and right dots, $${\mathrm{\Delta }}B_z^{{\mathrm{CR}}}$$, is designed to be ~40 mT (Supplementary Fig. 5b) to make the eigenstates of QST |↑↓〉 and |↓↑〉 rather than |S〉 and |T〉 by satisfying $${\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}} \gg J^{{\mathrm{ST}}}$$. Note that $${\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}} = |g|\mu _{\mathrm{B}}{\mathrm{\Delta }}B_z^{{\mathrm{CR}}}$$ where g~ −0.4 and μB are the electron g-factor and Bohr magneton, respectively. From the design we expect a large variation of $${\mathrm{\Delta }}B_z^{{\mathrm{CR}}}$$ when the electron in the center dot is displaced by the electric field. Indeed, we observe a strong influence of the gate voltages on $${\mathrm{\Delta }}B_z^{{\mathrm{CR}}}$$, which reaches ~100 mT $$\left( {{\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}}/h \sim 500\,{\mathrm{MHz}}} \right)$$ in the configuration chosen for the two-qubit gate experiment.

### Estimation of the ST precession parameters

Here we describe the estimation of the ST precession parameters in Eq. 2 under the influence of a fluctuating single-qubit phase of QST. Out of the parameters involved, $$\phi _{\sigma _z^{{\mathrm{LD}}}}$$ is the only parameter assumed to be QLD state-dependent, and the rest is classified into two types. One is the pulse-cycle-independent parameters, $$a,b,J^{{\mathrm{QQ}}},T_2^ \ast$$ and t0 which is constant during the experiment, and the other is the pulse-cycle-dependent parameters, $$\sigma _z^{{\mathrm{LD}}},{\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}}$$ and ϕ0, which can change cycle by cycle. Each pulse cycle consists of pulse stages from A to C as shown in Fig. 2b. We run the pulse cycle consecutively with a MW frequency fixed at 17.26 GHz and collect the data while QLD drifts between on-resonances and off-resonances with the MW burst due to the nuclear field fluctuation. To decrease the uncertainty of the estimated parameters, we choose the cycles during which the spin flip of QLD is unlikely in the following manner. The cycles throughout which QLD is likely to be |↓〉 are post-selected by the condition that QLD is on-resonance (i.e., Rabi oscillation of QLD is observed in ensemble-averaged data from nearby cycles) and the final state of QLD is measured to be |↓〉 at pulse stage C. Similarly, the cycles for QLD = |↑〉 are post-selected by the condition that QLD is off-resonance and the final state of QLD is measured to be |↑〉. The data structure and the index definitions for MLE are summarized in Supplementary Table 1. k is the index of the interaction time such that tint = 0.83 × k ns with k ranging from 1 to 100. m is the pulse-cycle index ranging from 1 (2001) to 2000 (4000) for QLD prepared in |↑〉 (|↓〉). The estimation procedure is the following. From all the readout results of QST (stage H) obtained in the cycles, we first estimate the five pulse-cycle-independent parameters by MLE. Note that JQQ may have a small pulse-cycle-dependent component due to charge noise but this effect is captured as additional fluctuation in $${\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}}$$ and ϕ0 in our model. We apply MLE to 100 × 4000 readout results of QST, $$r_m^k = 1$$ (0) for QST = |S〉 (|T〉). To this end, we first introduce the likelihood Pm defined in the eight dimensional parameter space as

$$P_m\left( {a,b,t_0,J^{{\mathrm{QQ}}},T_2^ \ast ,\sigma _z^{{\mathrm{LD}}},\phi _0,{\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}}} \right) = \mathop {\prod }\limits_{k = 1}^{100} \left( {r_m^kP_{{\mathrm{S}},{\mathrm{model}}} + (1 - r_m^k)(1 - P_{{\mathrm{S}},{\mathrm{model}}})} \right)$$
(3)

where PS,model is defined in Eq. (2). We calculate Pm on a discretized space within a chosen parameter range (Supplementary Table 2) using a single cycle data. Then we obtain Pm for the target five parameters as a marginal distribution by tracing out the pulse-cycle-dependent parameters,

$$P_{\mathrm{m}}\left( {a,b,t_0,J^{{\mathrm{QQ}}},T_2^ \ast } \right) = \mathop {\sum }\limits_{\sigma _z^{{\mathrm{LD}}}} \mathop {\sum }\limits_{\phi _0} \mathop {\sum }\limits_{{\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}}} P_m\left( {a,b,t_0,J^{{\mathrm{QQ}}},T_2^ \ast ,\sigma _z^{{\mathrm{LD}}},\phi _0,{\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}}} \right).$$
(4)

Repeating this process for all pulse cycles, we obtain the likelihood P as

$$P\left( {a,b,t_0,J^{{\mathrm{QQ}}},T_2^ \ast } \right) = \mathop {\prod }\limits_m P_m\left( {a,b,t_0,J^{{\mathrm{QQ}}},T_2^ \ast } \right).$$
(5)

We choose the maximum of P as the estimator for abt0, JQQ and $$T_2^ \ast$$, obtaining a = 0.218 ± 0.005, b = 0.511 ± 0.003, t0 = 1.53 ± 0.17 ns, JQQ/h = 90.2 ± 0.3 MHz, $$T_2^ \ast = 211 \pm 37$$ ns.

Once these values are fixed, we estimate the pulse-cycle-dependent parameters, $$\sigma _z^{{\mathrm{LD}}},\phi _0$$ and $${\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}}$$, for each cycle m. Note that $$\sigma _z^{{\mathrm{LD}}}$$ could be prepared deterministically if the state preparation of QLD were ideal, but here we treat it as one of the parameters to be estimated because of a finite error in the QLD state preparation. We again evaluate the likelihood $$P_m\left( {\sigma _z^{{\mathrm{LD}}},\phi _0,{\mathrm{\Delta }}E_{\mathrm{Z}}^{{\mathrm{ST}}}} \right)$$ defined in a discretized three dimensional space of its parameters using Eq. 3 and find their values that maximize the likelihood.

Based on the values of $$a,b,T_2^ \ast$$ and ϕST determined above, we can directly estimate $$\phi _{\sigma _z^{{\mathrm{LD}}}}$$ controlled by QLD for each tint without presumptions on the value of JQQ. To this end, we search for the parameter $$\phi _{\sigma _z^{{\mathrm{LD}}}}$$ that maximizes the likelihood

$$P^k\left( {\phi _{\sigma _z^{{\mathrm{LD}}}}} \right) = \mathop {\prod }\limits_m \left( {r_m^kP_{{\mathrm{S}},{\mathrm{model}}} + \left( {1 - r_m^k} \right)\left( {1 - P_{{\mathrm{S}},{\mathrm{model}}}} \right)} \right).$$
(6)

The obtained estimators for ϕ|↓〉 and ϕ|↑〉 are consistent with the expected values ±πJQQ(tint + t0)/h calculated from JQQ/h and t0 found above (see Fig. 3a).

The ensemble-averaged phase $$\left\langle {\phi _{\sigma _z^{{\mathrm{LD}}}}} \right\rangle$$ is obtained based on a similar estimation protocol. Here we estimate $$\phi _{\sigma _z^{{\mathrm{LD}}}}$$ for each m with fixed k = 5 (tint = 4.2 ns) to yield ϕC ≈ π from the likelihood $$P_m^{k = 5} = r_m^{k = 5}P_{{\mathrm{S}},{\mathrm{model}}} + \left( {1 - r_m^{k = 5}} \right)\left( {1 - P_{{\mathrm{S}},{\mathrm{model}}}} \right)$$ and then take the average of the estimated values for 800 pulse cycles. The oscillation visibility of $$\left\langle {\phi _{\sigma _z^{{\mathrm{LD}}}}} \right\rangle$$ in Fig. 4b is limited by three factors, low preparation fidelity of the input QLD state, estimation error of $$\phi _{\sigma _z^{{\mathrm{LD}}}}$$ and CPHASE gate error. The first contribution is likely to be dominant as the visibility of the oscillation in P is correspondingly low. Note that the effect of those errors is not visible in Fig. 3 because the most likely values of $$\phi _{\sigma _z^{{\mathrm{LD}}}}$$ are plotted.

## Data availability

The data that support the findings of this study are available from the corresponding authors upon reasonable request.

## References

1. Nielsen, M. A. & Chuang, I. L. Quantum Computation and Quantum Information. Cambridge Series on Information and the Natural Sciences (Cambridge University Press, Cambridge, UK, 2000).

2. Martinis, J. M. Qubit metrology for building a fault-tolerant quantum computer. npj Quantum Inf. 1, 15005 (2015).

3. Loss, D. & DiVincenzo, D. P. Quantum Computation with Quantum Dots. Phys. Rev. A 57, 120–126 (1998).

4. Koppens, F. H. L. et al. Driven coherent oscillations of a single electron spin in a quantum dot. Nature 442, 766–771 (2006).

5. Yoneda, J. et al. A quantum-dot spin qubit with coherence limited by charge noise and fidelity higher than 99.9%. Nat. Nanotechnol. 13, 102–106 (2018).

6. Zajac, D. M. et al. Resonantly driven CNOT gate for electron spins. Science 359, 439–442 (2017).

7. Watson, T. F. et al. A programmable two-qubit quantum processor in silicon. Nature 555, 633–637 (2018).

8. Veldhorst, M. et al. A two-qubit logic gate in silicon. Nature 526, 410–414 (2015).

9. Veldhorst, M. et al. An addressable quantum dot qubit with fault-tolerant control-fidelity. Nat. Nanotechnol. 9, 981–985 (2014).

10. Taylor, J. M. et al. Fault-tolerant architecture for quantum computation using electrically controlled semiconductor spins. Nat. Phys. 1, 177–183 (2005).

11. Petta, J. R. et al. Coherent manipulation of coupled electron spins in semiconductor quantum dots. Science 309, 2180–2184 (2005).

12. Barthel, C. et al. Rapid single-shot measurement of a singlet-triplet qubit. Phys. Rev. Lett. 103, 160503 (2009).

13. Nakajima, T. et al. Robust single-shot spin measurement with 99.5% fidelity in a quantum dot array. Phys. Rev. Lett. 119, 017701 (2017).

14. Shulman, M. D. et al. Demonstration of entanglement of electrostatically coupled singlet-triplet qubits. Science 336, 202–205 (2012).

15. Medford, J. et al. Self-consistent measurement and state tomography of an exchange-only spin qubit. Nat. Nanotechnol. 8, 654–659 (2013).

16. Elzerman, J. M. et al. Single-shot read-out of an individual electron spin in a quantum dot. Nature 430, 431–435 (2004).

17. Baart, T. et al. Single-spin CCD. Nat. Nanotechnol. 11, 330–334 (2016).

18. Mehl, S. & DiVincenzo, D. P. Simple operation sequences to couple and interchange quantum information between spin qubits of different kinds. Phys. Rev. B 92, 115448 (2015).

19. Trifunovic, L. et al. D. Long-distance spin-spin coupling via floating gates. Phys. Rev. X 2, 011006 (2012).

20. Yoneda, J. et al. Fast electrical control of single electron spins in quantum dots with vanishing influence from nuclear spins. Phys. Rev. Lett. 113, 267601 (2014).

21. Pioro-Ladrière, M. et al. Electrically driven single-electron spin resonance in a slanting Zeeman field. Nat. Phys. 4, 776–779 (2008).

22. Tokura, Y., van der Wiel, W. G., Obata, T. & Tarucha, S. Coherent Single Electron Spin Control in a Slanting Zeeman Field. Phys. Rev. Lett. 96, 047202 (2006).

23. Yoneda, J. et al. Robust micromagnet design for fast electrical manipulations of single spins in quantum dots. Appl. Phys. Express 8, 084401 (2015).

24. Reilly, D. J., Marcus, C. M., Hanson, M. P. & Gossard, A. C. Fast single-charge sensing with a rf quantum point contact. Appl. Phys. Lett. 91, 162101 (2007).

25. Barthel, C. et al. Fast sensing of double-dot charge arrangement and spin state with a radio-frequency sensor quantum dot. Phys. Rev. B 81, 161308(R) (2010).

26. Noiri, A. et al. Coherent electron-spin-resonance manipulation of three individual spins in a triple quantum dot. Appl. Phys. Lett. 108, 153101 (2016).

27. Barthel, C. et al. Relaxation and readout visibility of a singlet-triplet qubit in an Overhauser field gradient. Phys. Rev. B 85, 035306 (2012).

28. Nakajima, T. et al. Coherent transfer of electron spin correlations assisted by dephasing noise. Nat. Commun. 9, 2133 (2018).

29. Delbecq, R. M. et al. Quantum dephasing in a gated GaAs triple quantum dot due to nonergodic noise. Phys. Rev. Lett. 116, 046802 (2016).

30. Shulman, M. D. et al. Suppressing qubit dephasing using real-time Hamiltonian estimation. Nat. Comm. 5, 5156 (2014).

31. Martins, F. et al. Noise suppression using symmetric exchange gates in spin qubits. Phys. Rev. Lett. 116, 116801 (2016).

32. Reed, M. D. et al. Reduced sensitivity to charge noise in semiconductor spin qubits via symmetric operation. Phys. Rev. Lett. 116, 110402 (2016).

33. Nichol, J. M. et al. High-fidelity entangling gate for double-quantum-dot spin qubits. npj Quantum Inf. 3, 3 (2017).

34. Fowler, A. G., Mariantoni, M., Martinis, J. M. & Cleland, A. N. Surface codes: towards practical large-scale quantum computation. Phys. Rev. A 86, 032324 (2012).

35. Braginsky, V. B. & Khalili, F. Ya Quantum nondemolition measurements: the route from toys to tools. Rev. Mod. Phys. 68, 1–11 (1996).

36. Wardrop, M. P. & Doherty, A. C. Exchange-based two-qubit gate for singlet-triplet qubits. Phys. Rev. B 90, 045418 (2014).

Download references

## Acknowledgements

Part of this work is financially supported by the ImPACT Program of Council for Science, Technology and Innovation (Cabinet Office, Government of Japan), the Grant-in-Aid for Scientific Research (No. 26220710), CREST (JPMJCR15N2, JPMJCR1675), JST, Incentive Research Project from RIKEN. A.N. acknowledges support from Advanced Leading Graduate Course for Photon Science (ALPS). T.N. acknowledges financial support from JSPS KAKENHI Grant Number 18H01819. T.O. acknowledges financial support from Grants-in-Aid for Scientific Research (No. 16H00817, 17H05187), PRESTO (JPMJPR16N3), JST, The Telecommunications Advancement Foundation Research Grant, Futaba Electronics Memorial Foundation Research Grant, Hitachi Global Foundation Kurata Grant, The Okawa Foundation for Information and Telecommunications Research Grant, The Nakajima Foundation Research Grant, Japan Prize Foundation Research Grant, Iketani Science and Technology Foundation Research Grant,Yamaguchi Foundation Research Grant, Kato Foundation for Promotion of Science Research Grant. A.D.W. and A.L. acknowledge gratefully support of DFG-TRR160, BMBF - Q.Link.X 16KIS0867, and the DFH/UFA CDFA-05-06.

## Author information

Authors

### Contributions

A.N. and J.Y. conceived the experiment. A.N. and T.N. performed the measurement with the assistance of K.K., Y.K., M.R.D., T.O., K.T., S.A., and G.A. A.N. and T.N. conducted data analysis with the inputs from J.Y., P.S., and D.L. A.N. and T.N. fabricated the device on the heterostructure grown by A.L. and A.D.W. A.N. and T.N. wrote the manuscript with inputs from other authors. All authors discussed the results. The project was supervised by S.T.

### Corresponding authors

Correspondence to A. Noiri or S. Tarucha.

## Ethics declarations

### Competing interests

The authors declare no competing interests.

## Additional information

Publisher’s note: Springer Nature remains neutral with regard to jurisdictional claims in published maps and institutional affiliations.

## Rights and permissions

Open Access This article is licensed under a Creative Commons Attribution 4.0 International License, which permits use, sharing, adaptation, distribution and reproduction in any medium or format, as long as you give appropriate credit to the original author(s) and the source, provide a link to the Creative Commons license, and indicate if changes were made. The images or other third party material in this article are included in the article’s Creative Commons license, unless indicated otherwise in a credit line to the material. If material is not included in the article’s Creative Commons license and your intended use is not permitted by statutory regulation or exceeds the permitted use, you will need to obtain permission directly from the copyright holder. To view a copy of this license, visit http://creativecommons.org/licenses/by/4.0/.

Reprints and Permissions

## About this article

### Cite this article

Noiri, A., Nakajima, T., Yoneda, J. et al. A fast quantum interface between different spin qubit encodings. Nat Commun 9, 5066 (2018). https://doi.org/10.1038/s41467-018-07522-1

Download citation

• Received:

• Accepted:

• Published:

• DOI: https://doi.org/10.1038/s41467-018-07522-1

## Further reading

• ### Probabilistic teleportation of a quantum dot spin qubit

• Y. Kojima
• T. Nakajima
• S. Tarucha

npj Quantum Information (2021)

• ### Robust energy-selective tunneling readout of singlet-triplet qubits under large magnetic field gradient

• Wonjin Jang
• Jehyun Kim
• Dohun Kim

npj Quantum Information (2020)

• ### Quantum non-demolition readout of an electron spin in silicon

• J. Yoneda
• K. Takeda
• S. Tarucha

Nature Communications (2020)

• ### Quantum non-demolition measurement of an electron spin qubit

• Takashi Nakajima
• Akito Noiri
• Seigo Tarucha

Nature Nanotechnology (2019)

## Comments

By submitting a comment you agree to abide by our Terms and Community Guidelines. If you find something abusive or that does not comply with our terms or guidelines please flag it as inappropriate.

## Search

### Quick links

Sign up for the Nature Briefing newsletter — what matters in science, free to your inbox daily.

Get the most important science stories of the day, free in your inbox. Sign up for Nature Briefing