Electric field manipulation enhanced by strong spin-orbit coupling: promoting rare-earth ions as qubits

Abstract

Quantum information processing based on magnetic ions has potential for applications as the ions can be modified in their electronic properties and assembled by a variety of chemical methods. For these systems to achieve individual spin addressability and high energy efficiency, we exploited the electric field as a tool to manipulate the quantum behaviours of the rare-earth ion which has strong spin-orbit coupling. A Ce:YAG single crystal was employed with considerations to the dynamics and the symmetry requirements. The Stark effect of the Ce³⁺ ion was observed and measured. When demonstrated as a quantum phase gate, the electric field manipulation exhibited high efficiency which allowed up to 57 π/2 operations before decoherence with optimized field direction. It was also utilized to carry out quantum bang-bang control, as a method of dynamic decoupling, and the refined Deutsch-Jozsa algorithm. Our experiments highlighted rare-earth ions as potentially applicable qubits because they offer enhanced spin-electric coupling which enables high-efficiency quantum manipulation.

quantum coherent manipulation, spin-orbit coupling, spin-electric coupling, rare-earth ions, qubits

INTRODUCTION

Quantum computation offers accelerated ways of solving problems such as database searching [1] and prime factor decomposition [2]. Recently, there is an uprising trend to employ magnetic molecules as quantum bits (qubits), because of their advantages including monodispersed size and chemically controllable properties [3]. In these magnetic molecules where the electron spin is utilized, the electronic structure and quantum coherence are tunable by modifying the environment of the spin [4], and the dimension of the Hilbert space can be increased by designing the magnetic coupling between the spin carriers. The quantum phase memory time of the electron spin has been largely increased to nearly a millisecond by molecular design using nuclear spin-free ligands [5], indicating a bright future for quantum information processing based on electron spin qubits.

However, the magnetic field is hardly desirable when controlling electron spins in the quantum information processing context as the addressability of a single spin is difficult to realize because of the poor locality of the magnetic field. The electric field (E field), which can be much more concentrated and efficient, offers a promising alternative. Coupling between the E field and spins is referred to as spin-electric coupling and observed in the Stark effect. Related magnetic resonance research was first published in the 1960s [6,7], and later reviewed by Mims [8].

Electric control of spins has been proposed to realize electric dipole-induced spin resonance in semiconductors [9], and numerous experiments have been performed to control magnetic quantum dots [10], single electron spins [11], diamond defects [12] and the single nuclear spin in a molecular magnet [13]. Coherent control of an electron spin ensemble has been demonstrated in pnictogen-doped silicon semiconductors [14–16], piezo-diluted magnetic semiconductors [17] and molecular magnets [18]. Most recently, A. Morello and co-workers reported nuclear electric resonance using a high-spin ¹²³Sb nuclear doped in silicon, indicating the importance of electric control of the spin in quantum information processing [19].

The electric control of electron spin was not observed for some of the molecular magnets reported as qubits, and was observed to be inefficient in others, especially those with light elements. This is mainly because the spin-electric coupling is weak, and hinders their further application as qubits. The present study aims to solve this problem using rare-earth ions in a crystal. We report largely enhanced spin-electric coupling with which coherent control by the E field is illustrated as a phase gate. Using this electric phase gate, quantum bang-bang decoupling is realized with microwave (mw) pulses, and the refined Deutsch-Jozsa (D-J) algorithm is demonstrated.

Background: the role of spin-orbit coupling

The spin and orbital motions of electrons generate magnetic moments and contribute to a variety of spectroscopic and chemical phenomena. Unlike main group elements and transition metals, the orbital angular momentum in rare-earth ions originates from the inner subshell of 4f, and thus is unquenched by the crystal field, making the spin-orbit coupling dominate the properties of 4f electrons. In general, the Hamiltonian of a paramagnetic ion can be written as

$$\begin{equation}\hat{H} = {\mu _B}{{\boldsymbol B}^T} ({\hat{\boldsymbol L}} + {g_e}{\hat{\boldsymbol S}}) + \lambda {\hat{\boldsymbol L}^T} {\hat{\boldsymbol S}} + {\hat{H}_{\scriptsize\textit{CF}}},\end{equation}$$

(1)

where the three terms represent the Zeeman splitting, the spin-orbit coupling and the crystal field effect, the last of which results basically from the electrostatic field around the ion. The external E field Hamiltonian |${\hat{H}_E}$| can be viewed as a variation to the crystal field term arising from atomic displacements and charge redistribution. To the first order it can be expressed as |${\hat{H}_E} = \ ( {\partial {{\hat{H}}_{CF}}/\partial {E_x},\ \partial {{\hat{H}}_{CF}}/\partial {E_y},\ \partial {{\hat{H}}_{CF}}/\partial {E_z}} ) \cdot {^{^{\rightharpoonup}}}\hspace{-7.5pt}{E}$|⁠. In cases where the spin-orbit coupling can be treated as a perturbation, the above Hamiltonian can be converted and expressed in the spin operator only, as

$$\begin{equation}\hat{H} = {\mu _B}{\boldsymbol B}^{T} \overline{\overline {\boldsymbol{g}}} \hat{\boldsymbol S} + {\hat{\boldsymbol S}^T}\overline{\overline {\boldsymbol{D}}} \hat{\boldsymbol S},\end{equation}$$

(2)

where |$\overline{\overline {\boldsymbol{g}}} = {g_e}\;\overline{\overline {\bf 1}} + 2\lambda \overline{\overline {\boldsymbol \Lambda} } ,\;\overline{\overline {\boldsymbol{D}}} = {\lambda ^2}\overline{\overline {\boldsymbol{\Lambda }}} ,{\rm{and}}\;\overline{\overline {\boldsymbol{\Lambda }}} $| is a 3 × 3 matrix containing the orbital angular momentum eigenstates and their energies determined by the crystal field term. The effect of |${\hat{H}_E}$| is then included via |$\overline{\overline {\boldsymbol{\Lambda }}} $| in both the Zeeman and zero-field splitting terms and scales up with |$\lambda$|⁠. Cases with weak crystal field and strong spin-orbit coupling require more complicated theoretical treatments, but a similar basic principle still holds, indicating that strong spin-orbit coupling is desirable in seeking materials for efficientEfield control of a spin system. A recent study concluded that, with similar structures, spin-orbit coupling is not the primary factor leading to decoherence [20]. This ensures the possibility of employing strong spin-orbit coupling systems as qubits while maintaining long quantum coherence time. We therefore propose that rare-earth ions are desirable for strong spin-electric coupling.

The Stark effect has been observed in several bulk systems including pnictogen-doped silicon semiconductors [16] and piezoelectric materials [17], where the spin-orbit coupling of the spin carriers is weak, but the applied E field dramatically redistributes the electron wave function. In contrast, in the present study, the E field is used to manipulate the quantum coherence properties of the spins localized on the rare-earth ions individually.

Spin-orbit coupling may also help via spin-spin coupling. Antisymmetric exchange, also known as the Dzyaloshinskii-Moriya (D-M) interaction, arises from the electron spin anisotropy as a result of large spin-orbit coupling. This kind of exchange results in spin canting and net electric polarization, which provides strong spin-electric coupling. R. Sessoli and co-workers tuned the magnetic interaction between an organic radical and a Mn²⁺ ion in a single crystal in a chiral space group [21]. By applying the ac E field to the sample continuously, the electron paramagnetic resonance (EPR) spectra showed a shift of the effective g-factor up to −2.5 × 10⁻⁶.

RESULTS AND DISCUSSION

Observation of the spin-electric coupling

The Stark effect can be observed with two methods. A straightforward method is to apply the E field to the sample continuously to modify the energy levels of the spin carrier. The slight influence can be observed with a strong dc E field or, via signal modulation, with an ac E field. Another approach, which is more efficient and common for molecular magnets, is to measure via quantum phase evolution with pulsed EPR [18].

Previous researches using pulsed EPR were performed with powder samples. To evaluate the spin-electric coupling in more detail, a single crystal was used in our experiments. The emergence of the Stark effect in magnetic resonance requires that the spin carriers must not be located at any inversion centre. On the other hand, the number of inequivalent parameters needed to model the effect would be smaller if the spin centres were of higher symmetry. Based on these considerations, a yttrium aluminium garnet (YAG) single crystal doped with Ce³⁺ was employed. YAG crystallizes in the space group |$Ia\bar{3}d$| with cubic unit cells. Ce³⁺ was doped into the YAG crystal at the Y³⁺ positions [22]. There are six magnetically inequivalent sites [23] and each Ce³⁺ is identically coordinated by eight oxygen atoms with a local symmetry of D₂. The three C₂ axes serve as principal axes for the g-factor. Ce³⁺ ions appear in inversion pairs as a result of the central symmetry of the crystal (Fig. 1a). To eliminate the electron spin dipolar interactions, the concentration of Ce³⁺ ions was reduced to less than 0.1%, and the average distance between Ce³⁺ ions was more than 3 nm. To enhance the E field strength and acquire a significant signal, the Ce:YAG single crystal was cut to 0.5 mm in thickness, with a 2 × 6 mm² area to fit the sample into the cavity. The crystal was mounted so that the (111) face was perpendicular to the E field and parallel with the B₀ field. This geometry was fixed for all our experiments.

The Ce:YAG crystal structure and the device used in our experiments. (a) Locations of the six magnetically inequivalent Ce3+ ions marked Ce-1 to Ce-6. Each Ce3+ is coordinated by eight oxygen atoms. Their principle axes are shown as coloured arrows (red, green and blue for x, y and z, respectively). Inversion centres are located at (0.5, 0.5, 0.5) and (0.5±0.25, 0.5±0.25, 0.5±0.25). The inversion pairs involving Ce-1 to Ce-6 generated by (0.5, 0.5, 0.5) are also shown. (b) Ce:YAG single crystal of size 2 × 6 × 0.5 mm3 is mounted on the electrode, and connected to 0.2 mm gold wires with a 50 Ω match resistor.

Figure 1.

The Ce:YAG crystal structure and the device used in our experiments. (a) Locations of the six magnetically inequivalent Ce³⁺ ions marked Ce-1 to Ce-6. Each Ce³⁺ is coordinated by eight oxygen atoms. Their principle axes are shown as coloured arrows (red, green and blue for x, y and z, respectively). Inversion centres are located at (0.5, 0.5, 0.5) and (0.5±0.25, 0.5±0.25, 0.5±0.25). The inversion pairs involving Ce-1 to Ce-6 generated by (0.5, 0.5, 0.5) are also shown. (b) Ce:YAG single crystal of size 2 × 6 × 0.5 mm³ is mounted on the electrode, and connected to 0.2 mm gold wires with a 50 Ω match resistor.

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Figure 2.

Spin echo oscillation upon the application of an E field. (a) The pulse sequence employed in the experiment. The rectangular E field pulse is applied between the mw π/2 and π pulses of the standard Hahn echo pulse sequence. (b) The transient spin echo oscillates with increasing frequencies upon enhancing the E field strength from 0 to 10⁶ V/m. (c) The quantum phase evolution frequency, derived from the Fourier transformation of (b), shows a linear dependence on the E field strength. The error bars lie within the size of the points. (d) The quantum phase evolution frequency is simulated with varying directions of the E and B₀ fields. The most efficient frequency for quantum phase control is optimized to be 0.96 MHz when E//z and B₀//(0.44, 0.90, 0) with respect to the local Ce³⁺ coordinates. θ and φ denote the polar and azimuthal angles. The experiment was conducted at 10 K, with the microwave frequency 9.667 GHz.

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With strong spin-orbit coupling, the Ce³⁺ with 4f¹ electron configuration presents a J = 5/2 state. As a result of the large crystal field splitting, only the ground doublets can be observed in X-band EPR measurements. For simplicity, an effective spin 1/2 model is used, where the values of the highly anisotropic g-tensor depend on the crystal field parameters. Hence, the spin-electric coupling, enhanced by large spin-orbit coupling and significantly influencing the crystal field parameters, can be detected through the g-factor shift in our experiments.

In this model, the Hamiltonian of the Ce³⁺ ion in the external static magnetic field is |$\hat{H} = {\mu _{\boldsymbol B}}\ {\boldsymbol B}^{T}\overline{\overline {\boldsymbol g}} \hat{\boldsymbol S}$|⁠. By cw-EPR measurements and simulations, the principal values of the g-tensor are determined to be g_xx = 1.85, g_yy = 0.90 and g_zz = 2.74, which agree with the previous report [23].

We applied the E field pulse between the two mw pulses in the standard Hahn echo sequence (Fig. 2a). An oscillation of the spin echo can be observed when the duration of the E field pulse is increased, indicating a continuously changing quantum phase, as shown in Fig. 2b. This phase evolution can be used to characterize the Stark effect. The effect of the E field is mainly modifying the Zeeman splitting term, so we can generally express the Stark effect Hamiltonian as

$$\begin{equation}{\rm{\ }}{\hat{H}_E} = \mathop \sum \limits_{ijk} {E_i}{T_{ijk}}{\mu _B}{B_j}{\hat{S}_k}{\rm{}},\end{equation}$$

(3)

where |${T_{ijk}} = {\rm{\ }}\partial {g_{jk}}/\partial {E_i}$| are components of the Stark effect tensor regarding different directions. The D₂ local symmetry of Ce³⁺ will eliminate most of them and merge the others into three, giving

$$\begin{eqnarray} {\hat{H}_E} &=& {\mu _B}{\rm{\ }}\big[ {E_x}{T_{xyz}}\left( {{B_y}{{\hat{S}}_z} + {B_z}{{\hat{S}}_y}} \right)\nonumber\\ +\, {E_y}{T_{yxz}}\left( {{B_x}{{\hat{S}}_z} + {B_z}{{\hat{S}}_x}} \right) \nonumber\\ +\, {E_z}{T_{zxy}}\left( {{B_x}{{\hat{S}}_y} + {B_y}{{\hat{S}}_x}} \right) \big], \end{eqnarray}$$

(4)

where parameters |${T_{xyz}}$|⁠, |${T_{yxz}}$| and |${T_{zxy}}$| can be determined by detecting the phase evolution with different applied E fields, as detailed in SI. In our work, five different amplitudes from 0 to 10⁶ V/m were applied to the Ce:YAG single crystal. It can be clearly seen that the spin echo phase evolution frequency showed a linear response to the external E field, as shown in Fig. 2c. It is worth noting that the rising and falling edges of the E field pulse are about 40 ns. The induced magnetic field is at the mG level, comparable to the static and dynamic inhomogeneity from the magnet providing the external magnetic field (B₀ field) in the spectrometer, and thus is neglected.

It is important to quantify the effect to optimize the manipulation speed of this quantum phase gate. The Stark effect shows strong anisotropy when the E field pulse is applied in different directions in the Ce³⁺ local coordinate system. By fitting the four experimental curves with a calculated formula, the parameters are determined to be |${T_{xyz}} = \ 3.30( 2 )\ \times {10^{ - 8}}\ {\rm{m}}/{\rm{V}}$|⁠, |${T_{yxz}} = \ 8.76( 6 )\ \times {10^{ - 8}}\ {\rm{m}}/{\rm{V}}$| and |${T_{zxy}} = \ 12.1( 1 )\ \times {10^{ - 8}}\ {\rm{m}}/{\rm{V}}$|⁠. This measurement, as well as all below, was conducted at 10 K.

With this set of parameters, we can optimize the efficiency of the E field used to manipulate the spin quantum phase. As the Stark effect is highly anisotropic, we can find the directions of the E field and the B₀ field in the Ce³⁺ local coordinates that give the largest coupling strength. Through simulation, a coupling constant of 1.6 MHz·m/(T·MV) is acquired when the B₀ field is along (0.44, 0.90, 0) and the E field is along (0, 0, 1) in the Ce³⁺ local coordinates as shown in Fig. 2d. With |$E\ = \ 1\ {\rm{MV}}/{\rm{m}}$| and |${B_0} = \ 0.6\ {\rm{T}}$|⁠, the coupling efficiency can be enhanced to 0.96 MHz with proper orientation.

Different from the effect of crystal-field and hyperfine-coupling terms, the energy shift induced by the E field, originating from the Zeeman term, is proportional to the B₀ field, as in Eq. 3. Therefore, the manipulation efficiency of this E field pulse can be enhanced by increasing the B₀ field. A strongB₀ field provides plenty of other advantages, e.g. resolution enhancement, a high-quality initialized state, and a long phase memory time [24]. Conclusively, in the present research, it is safe to work with a relatively weak E field.

Electric field as a phase gate

The above Stark effect experiment highlights some important information about the quantum state manipulation of Ce:YAG. This controllable effect could lead to an effective phase evolution. By applying the E field pulse between the two mw pulses, the spin echo could gain an additional phase factor, which is controlled by both the E field strength and the duration. Normally, mw pulses for electron spin manipulations are tens of nanoseconds in length. In our experiments, by optimizing the operating conditions of the E field pulse, a π/2 phase evolution can be shortened to within 260 ns. In contrast, the phase memory time of Ce:YAG at 10 K is measured to be up to 15 μs. This results from the relatively high symmetry and the almost spin-free surrounding oxygen nuclei. A useful characterization of a qubit is its maximal number of effective operations before decoherence. In this research, a sequence of up to 57 π/2 rotations is allowed before the system decoheres. In quantum information processing, an E field pulse can be considered as a quantum phase gate

$$\begin{equation}\hat{R} \left( \phi \right) = {e^{ - i{{\hat{H}}_E}t}}\ = \left( {\begin{array}{@{}*{2}{c}@{}} {{e^{ - i\phi /2}}}&\quad 0\\ 0&\quad {{e^{i\phi /2}}} \end{array}} \right),\end{equation}$$

(5)

which offers an additional phase difference |${e^{i\phi }}$|⁠.

This efficient quantum phase evolution offers us the possibility of demonstrating several quantum manipulations by the E field. Because of the higher operating rate, we can use the mw pulse to reverse the phase factor while the electron spin is undergoing the evolution in the external E field. In this demonstration, the electron spin is firstly prepared in a superposition state in the xy plane of the Bloch sphere by a mw pulse. Then the E field pulse could drive phase evolution of this superposition state, as if there were an additional magnetic field along the z axis. During this evolution driven by the E field, the system can be ‘kicked’ by short mw π pulses to another state within the xy plane. Based on the pulse sequence used in the former experiment in Stark effect detection, these microwave π pulses were added symmetrically about the π pulse in the Hahn-echo sequence. During the E field pulse, a series of mw π pulses at arbitrarily chosen moments were applied to reverse the evolution of the spin polarization, as shown in Fig. 3a. This kind of operation is similar to the experiments with fullerene qubits [25]. The spin polarization evolves in the xy plane under the E field, while a mw π pulse drives the spin rapidly around the B₁ field along a half-circle, as illustrated in Fig. 3b.

Figure 3.

The E field phase gate demonstration of quantum bang-bang control and the dynamic decoupling realized by mw pulses. (a) (I) The phase evolution within the xy plane of the Bloch sphere driven by theE field phase gate. (II) to (V), Four trains of mw pulses to kick the spin echo. The arrows indicate the moment at which the mw pulses are applied. The quantum phase evolution reverses when applying the microwave pulses. (b) The Bloch sphere demonstration of this bang-bang control. The bold purple curve represents the spin phase evolution induced by the E field phase gate, and the thin green curves indicate the mw ‘kicking’ operation. The straight red arrow is the B₁ field direction. (c) Successive mw pulses, which were continuously implemented during the plateaus, can lock and release the phase evolution at arbitrary positions. The experiment was conducted at 10 K, with the microwave frequency 9.667 GHz.

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In the above demonstration, the mw pulses operate much faster than the E field pulses. In the original proposal of bang-bang control, rapid spin flips are employed by short mw pulses to prevent the unwanted phase evolution [26]. As in Fig. 3c, when the system evolves in the xy plane driven by the E field and a series of mw π pulses is applied, one can see that the spin evolution is locked, and the spin is decoupled from the E field during the mw pulses. This is an example of the quantum Zeno effect, in which the quantum phase evolution is supressed by repeated measurements or controllable interactions with the environment [27]. The spin evolution is released at the end of each mw pulse, which can be locked again by the next. It is necessary to mention that, unlike the projective quantum Zeno effect experiment which locks the system in the eigenstate [28], this experiment can lock the system in any state.

Phase gate application: D-J algorithm

This efficient quantum phase gate could also help to demonstrate the refined D-J algorithm. The D-J problem is to determine whether a given oracle function |$f\!\!:{\rm{}}{\{ {0,1} \}^n} \to \{ {0,1} \}$|⁠, which takes an n-digit binary input and produces 0 or 1 as the output, is a balanced function (0 for half of the inputs and 1 for the other half) or a constant function (uniformly 0 or 1 for all inputs). A classical computer requires |${2^{n - 1}} + 1$| times of evaluation to solve this problem for the n-bit input situation, whereas quantum computing can solve it in a single try. This has been achieved with ¹⁹F nuclear spins [29], but not yet with electron spins. A refined version of the D-J algorithm proposed by D. Collins and co-workers uses one of the input qubits as the output, allowing the n-bit problem to be solved using n qubits [30]. Two types of quantum phase gates are required in our demonstration of the refined D-J algorithm with |$n\ = \ 1$|⁠. The first, the Hadamard gate regarding the basis set |$|\ {s_z} = \ \pm 1/2 \rangle$|⁠, which can be performed by a π/2 mw pulse, is used to generate a uniform superposition of the two possible inputs and to convert the output to a readable eigenstate in the end. The second, the f-controlled control gates are used to encode the functions for calculation. Here, the algorithm can be demonstrated in this two-level system with the E field quantum phase gate with a field strength of |$0.8\ \times {10^6}$| V/m.

There are only four possible oracle functions for the single input situation in the D-J problem: |${f_1} (x) = 0$|⁠, |${f_2}\! (x) = 1$|⁠,|${f_3}\! (x) = 1 - x$| and |${f_4}\! (x) = x$|⁠. These four functions can be encoded as 4 f-controlled gates realized by:

${U_{\!\!{f_1}}} = ({\begin{array}{@{}*{2}{c}@{}}{1}\,\,\,{0}\\{0}\,\,\,{1} \end{array}}) = \hat{R}\!(0)$

⁠,

${U_{\!\!{f_2}}} = ( {\begin{array}{@{}*{2}{c}@{}}{{ - 1}}\,\,\,{0}\\{0}\,\,\,{{ - 1}} \end{array}} )= \hat{\!{R}}( {2\pi } )$

⁠,

${U_{\!\!{f_3}}} \!=\! ( {\begin{array}{@{}*{2}{c}@{}}{{ - 1}}\,\,{0}\\{0}\,\,{1} \end{array}} ) \!=\! \hat{\!{R}}( \pi )$

and

${U_{\!\!{f_4}}} \!=\! ( {\begin{array}{@{}*{2}{c}@{}}{1}\,\,{0}\\{0}\,\,{{ - 1}} \end{array}} )\! =\! \hat{\!{R}}( { - \pi })$

⁠. The superposition state |$\frac{1}{{\sqrt 2 }}( {| {0 \rangle + } |1 \rangle} )$| generated by the first Hadamard gate is transformed to |$\frac{1}{{\sqrt 2 }}[ {{{( { - 1} )}^{{f_i}( 0 )}}| {0 \rangle + {{( { - 1} )}^{{f_i}( 1 )}}} |1} \rangle ]$| by |${U_{\!{f_i}}}$|⁠, and then transformed to |$|0 \rangle $| or |$|1 \rangle $| by the π pulse and the second Hadamard gate for readout. The final Hahn echo is detected as the result, which can be |$|0 \rangle $| (for constant functions, |${f_1}$| and |${f_2}$|⁠, Fig. 4b and c) or |${|1 \rangle}$| (for balanced functions, |${f_3}$| and |${f_4}$|⁠, Fig. 4d and e). Unlike the previously reported implementation of the D-J algorithm in the diamond NV-centre [31], for which the phase shift was achieved by an auxiliary state via a 2π rotation, in this research, the phase shift gate is realized by the electric phase gate, and only a two-level system is necessary.

$The refined D-J algorithm (n = 1) using the E field pulses as the f-controlled gates. (a) The pulse sequence of the D-J algorithm demonstration. The initial π/2 pulse is applied to prepare the superposition state of $\frac{1}{{\sqrt 2 }}( {| {0 \rangle + } |1 \rangle} )$. The green blocks indicate the four f-controlled gates, as shown in the insets of (b–e). The following π/2 pulse is to convert the evolved superposition state into eigenstates ${|0 \rangle}$ (for constant functions, ${f_1}$ and ${f_2}$) or ${|1 \rangle}$ (for balanced functions, ${f_3}$ and ${f_4}$). The final Hahn echo pulse sequence is to read out the eigenstates ${|0 \rangle}$ or ${|1 \rangle}$. The spin echo results are shown in (b–e), among which (b) and (c) with positive phases correspond to eigenstate ${|0 \rangle}$, whereas (d) and (e) with negative phases indicate eigenstate ${|1 \rangle}$. The experiment was conducted at 10 K, with the microwave frequency 9.667 GHz.$

Figure 4.

The refined D-J algorithm (n = 1) using the E field pulses as the f-controlled gates. (a) The pulse sequence of the D-J algorithm demonstration. The initial π/2 pulse is applied to prepare the superposition state of |$\frac{1}{{\sqrt 2 }}( {| {0 \rangle + } |1 \rangle} )$|⁠. The green blocks indicate the four f-controlled gates, as shown in the insets of (b–e). The following π/2 pulse is to convert the evolved superposition state into eigenstates |${|0 \rangle}$| (for constant functions, |${f_1}$| and |${f_2}$|⁠) or |${|1 \rangle}$| (for balanced functions, |${f_3}$| and |${f_4}$|⁠). The final Hahn echo pulse sequence is to read out the eigenstates |${|0 \rangle}$| or |${|1 \rangle}$|⁠. The spin echo results are shown in (b–e), among which (b) and (c) with positive phases correspond to eigenstate |${|0 \rangle}$|⁠, whereas (d) and (e) with negative phases indicate eigenstate |${|1 \rangle}$|⁠. The experiment was conducted at 10 K, with the microwave frequency 9.667 GHz.

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CONCLUSION

We have demonstrated that an E field pulse applied to the Ce:YAG can be a highly efficient quantum phase gate. The phase gate is utilized to perform quantum bang-bang control and the refined Deutsch-Jozsa algorithm. The example of Ce³⁺ with 4f¹ configuration showed that rare-earth ions, with the aid of a proper symmetry, can enhance the spin-electric coupling via their strong spin-orbit interaction. The optimized manipulation condition with the X-band frequency and 10⁶ V/m field strength allows over 50 π/2 phase gate operations within the phase memory time of up to 15 μs at 10 K. The application of E field quantum phase gates allows for achieving effective manipulations on the rare-earth qubit.

We would like to highlight the importance of spin-orbit coupling in the research on the E field coupling with the spin centre. The manipulation in our experiments, resulting from the strong spin-orbit coupling of the rare-earth ion, is much more efficient compared to those with other separated electron spin centres. The quantum coherence time, of course, is still an important factor to determine whether any application is possible, but faster manipulations allow us to be less picky about this. The E field in our experiments cannot exceed 10⁶ V/m because of the sample size, setting a limit to the maximal number of manipulations before decoherence. The 1 MHz coupling constant might be enhanced further in other setups such as single spin break-junction devices, where the E field can easily reach 10⁸ V/m with a few volts. Such an E field is focused enough to control the electron spin individually.

Shortly after an earlier version of our manuscript was submitted to arXiv [32], a work by J.-J. Liu and co-workers was published investigating the E field effect on the quantum coherence involving a clock transition in the HoW₁₀ molecular nanomagnet, which provides a platform with even longer phase memory time for operation [33]. With other advantages of rare-earth ions such as ultralong optical coherence times, optical readout [34,35], and the possibility of device fabrication by chemical modifications and assembly, the high-efficiency quantum phase gate achieved with enhanced spin-electric coupling in this research indicates that electron spin qubits based on rare-earth ions make promising candidates for quantum information processing towards application.

FUNDING

This work was supported by the National Basic Research Program of China (2018YFA0306003 and 2017YFA0204903), the National Natural Science Foundation of China (21822301, 11805024 and 11847301) and the Beijing Academy of Quantum Information Sciences (Y18G23).

AUTHOR CONTRIBUTIONS

Z.L. performed the measurements, assisted by Y.-X.W. and Y.-H.F. Z.L. and S.-D.J. processed the data and performed theoretical analysis. S.-X.Q. provided the methods to simulate the spin evolutions. Z.-M.W. performed the single crystal face index. The project was conceived by S.G. and S.-D.J. Z.L. and S.-D.J. designed the experiments and wrote the manuscript, assisted by Y.-X.W. All the authors revised the manuscript.

Conflict of interest statement. None declared.

REFERENCES

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Quantum mechanics helps in searching for a needle in a haystack

Phys Rev Lett

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Article Contents

Electric field manipulation enhanced by strong spin-orbit coupling: promoting rare-earth ions as qubits Open Access

Abstract

INTRODUCTION

Background: the role of spin-orbit coupling

RESULTS AND DISCUSSION

Observation of the spin-electric coupling

Electric field as a phase gate

Phase gate application: D-J algorithm

CONCLUSION

FUNDING

AUTHOR CONTRIBUTIONS

REFERENCES

Supplementary data

Citations

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Electric field manipulation enhanced by strong spin-orbit coupling: promoting rare-earth ions as qubits