Abstract
Spin echo is a fundamental tool for quantum registers and biomedical imaging. It is believed that a strong magnetic field is needed for the spin echo to provide long memory and high resolution, since a degenerate spin cannot be controlled or addressed under a zero magnetic field. While a degenerate spin is never subject to dynamic control, it is still subject to geometric control. Here we show the spin echo of a degenerate spin subsystem, which is geometrically controlled via a mediating state split by the crystal field, in a nitrogen vacancy centre in diamond. The demonstration reveals that the degenerate spin is protected by inherent symmetry breaking called zerofield splitting. The geometric spin echo under zero field provides an ideal way to maintain the coherence without any dynamics, thus opening the way to pseudostatic quantum random access memory and noninvasive biosensors.
Introduction
Nitrogen vacancy (NV) centres in diamond provide promising platforms for quantumrelated technologies. The coherence time of an electron spin in an NV centre has been shown to reach millisecond order even at room temperature^{1,2,3,4}. Arbitrary state preparation, single/twoqubit control, entanglement generation^{5,6,7} and quantum teleportation^{8} have also been achieved using the NV spin together with proximate nuclear spins. Quantum memory, however, must possess two contradictory qualities: noise resilience and controllability. Symmetric states are known to be fragile by themselves but become noise resilient with specific symmetrybreaking operations. Such symmetry breaking inherently occurs in an NV centre, where the groundstate electrons form triplet states with spin1 angular momentum. The zerofield splitting due to the spinspin interaction breaks the symmetry to push only the magnetic quantum number m_{S}=0 state far below the degenerate m_{S}=±1 states^{9}. The zerofield split state provides a dynamic path to manipulate the geometric phase of the logical qubit based on the m_{S}=±1 states^{10,11}. The same situation is seen in photon polarization^{12,13}, which is also spanned by degenerate m_{S}=±1 states representing circular polarizations with spin1 angular momentum. This correspondence allows spontaneous entanglement generation^{14} and entangled absorption^{15} between single photon and electrons in an NV centre in diamond. The correspondence also allows a microwave to be applied to manipulate an electron spin ±1 subsystem with arbitrary polarizations^{16}. Even when the subsystem is degenerate enough to avoid a field to drive the state, it is possible to geometrically control^{17,18} the geometric phase or the Berry phase^{19}. Geometric gate operation has been proposed for performing holonomic quantum computation with builtin noise resilience^{20,21,22,23}. The geometric phase has been experimentally observed in molecular ensembles^{24,25}, in a single superconducting qubit^{26}, and in a single NV centre in diamond^{10,11}. It has been shown that the geometric phase gate offers fast and precise control over the geometric phase, disrupts environmental interaction with multiple pulse echo sequences^{17}, and even offers a universal set of quantum logic gates^{10}.
Although those demonstrations introduced an energy gap to the qubit for controllability, here we show that it is possible to control a degenerate logical qubit, which we call a geometric spin qubit, by a purely geometric gate operation and that it can be protected by zerofield splitting with the help of a timereversal operation, which we call geometric spin echo.
Results
System and scheme
Our experimental demonstration of geometric spin control is based on the application of resonant microwave to electron spin in a diamond NV centre under a zero magnetic field. The electron spin system in an NV centre is described by the following Hamiltonian.
where S=(S_{x,}S_{y,}S_{z}) is the spin1 operator of the vacancy electron spin, I_{z} is the z component of the spin1/2 operator of the ^{14}N nuclear spin, D=(2π × )2.87 GHz is the axial zerofield splitting, E_{x} (E_{y}) is the x (y) component of the transverse zerofield splitting caused by a crystal strain, γ_{e} is the gyromagnetic ratio of the electron spin, B_{ext} is the external magnetic field and A_{z}=−(2π × )2.175 MHz is the z component of the hyperfine interaction between the electron spin and the ^{14}N nuclear spin. The x, y components of the hyperfine interaction and magnetic field, which contribute to the secondorder perturbation, are negligible owing to the large zerofield splitting. Note that in this paper we omit the Planck constant ħ for simplicity.
If we take only the first term of equation (1) as a dominant term, the ground state forms triplet states consisting degenerate states, which serve as logical qubit basis states, and a zerofield split state, which serves as an ancillary state for the geometric operation as shown in Fig. 1a. On the basis of the Jaynes–Cummings model, qthe interaction Hamiltonian with a microwave resonant to the energy gap between and states is described as , where Ω(t) denotes the Rabi frequency. We define the polarization of the microwave as a linear polarization oriented towards +x. The spin 1 operator indicates the state exchange between the bright state and , while the dark state remains unchanged (Fig. 1b). After a round trip time T, defined as , the bright state evolves as , where denotes the Pauli operator in the subspace. Note that the prefactor −1 is nothing but a global phase in the subspace, whereas in the subspace the global phase serves as a relative phase called the geometric phase for a geometric spin qubit. This geometric operation is represented as a π rotation around the axis or the x axis in the subspace as as shown in Fig. 1c. The pulse sequences used in the demonstrations are summarized in Fig. 1d (Methods).
Rabi oscillation and Ramsey interference
A series of experiments for calibrating the condition to achieve the geometric spin echo are performed under a zero magnetic field. The Rabi oscillation experiment determines the π pulse width required to flip the spin states between the state and the state (Fig. 2a). The oscillation conforms to the theory considering hyperfine coupling between the electron spin at the vacancy and the nuclear spin at the nitrogen (^{14}N) that comprises the NV. The Ramsey interference experiment or the freeinduction decay indicates that the hyperfine coupling induces electron spin precession to alter and states at a frequency corresponding to twice the hyperfine coupling (Fig. 2b). The Gaussian decay of the envelope indicates the geometric spin coherence time T_{2}* to be 0.61 μs. The origin of the decoherence would be the coupling of the electron spin to a spin bath consisting the proximate nuclear spins of the ^{13}C isotopes.
Geometric spin echo
The disappeared Ramsey interference signal seen in Fig. 2b recovers as a geometric spin echo by the insertion of 2π pulse after 35 μs of time evolution, and the signal reaches a maximum when the second evolution time equals the first (Fig. 3a). The result indicates that the geometric spin echo rephases the geometric spin as the conventional Hahn echo does the dynamic spin, even under complete degeneracy of the qubit space. Figure 3b shows the signal decay of the geometric spin echo under external magnetic fields of 0 mT (red squares), 0.04 mT (green circles) and 0.12 mT (blue triangles) measured along the NV axis. The coherence time is extended by the echo process to T_{2}=83 μs under a zero magnetic field, which is about 140 times longer than the T_{2}* of 0.61 μs. The echo coherence time drastically increases as decreasing the magnetic field from 0.12 mT, within which both of the Zeemansplit electron spin states are equally driven by the microwave. The T_{2} in Fig. 3b is determined only by fitting with under the assumption that the population decay behaves as , where T_{1}=700 μs is dominated by green laser leakage (Supplementary Fig. 1).
The echo coherence time T_{2} as a function of an external magnetic field measured along the NV axis (Fig. 3c) agrees relatively well with theory based on the disjoint cluster method^{27}, which neglects electron spin flip owing to the large axial zerofield splitting^{28}, for a spin bath consisting ^{13}C isotopes with a natural abundance of 1.1% (Methods). Single and dimer ^{13}C nuclear spins (nearestneighbour nuclear spin pair) were taken into account as bath spins but the interaction between bath spins were neglected^{29}.
Figure 4a decomposes contributions of single and dimer nuclear spins to the decoherence. Note that the single nuclear spins dominate decoherence under relatively high magnetic field, while the dimer nuclear spins dominate under a zero magnetic field. In the case of single nuclear spins, the quantization axis defined by the electron spin hyperfine field is deviated by the external magnetic field. In the other case of dimer nuclear spins, the quantization axis is deviate by the dipolar magnetic field within the dimer (Fig. 4b). In any case, the electron spin inversion in the logical qubit space cannot completely time reverse the nuclear spin dynamics during the geometric spin echo. In other words, the time evolution operators with orthogonal electron spin states become incompatible or irreversible by the additional field as in equation (9).
Discussions
The deviation from the theory around 0 and 0.075 mT in Fig. 3c, on the other hand, is explained by the strain, or the transverse zerofield splitting, which couples the otherwise degenerate m_{S}=±1 states to lift the degeneracy and further decouples the spin bath from the electron spin. The magnetic field to give maximum deviation 0.075 mT corresponds to the nitrogen hyperfine splitting 2.18 MHz. The range of the deviation ∼0.02 mT is explained by considering the strain splitting 0.23 MHz and inhomogeneous broadening 0.43 MHz of the optically detected magnetic resonance (ODMR) spectrum (Supplementary Fig. 3). The calculated magnetic field dependence of the echo T_{2} with the strain correction (Supplementary Fig. 3) agrees well with the experiments, indicating that the geometric spin qubit is protected against decoherence not only by the axial zerofield splitting but also by the transverse zerofield splitting. In contrast that the axial zerofield splitting suppresses the transverse hyperfine interaction, which causes a bitflip error to the secondorder perturbation, the transverse zerofield splitting suppresses the axial hyperfine interaction, which causes a phaseflip error , to the secondorder perturbation^{30}.
Although the achieved geometric echo coherence time T_{2} of 83 μs at the degeneracy is 140 times longer than the freeinduction decay of 0.61 μs, it is several times shorter than the measured population decay time T_{1} of 700 μs for the geometric spin state relaxing from to (Supplementary Fig. 1). The discrepancy between T_{1} and T_{2} can be compensated by excluding the effect of dimers not only by decreasing the abundances of ^{13}C isotopes but also by suppressing dimers into their singlet state to be spin transparent. Since the common dynamical qubit defined in the 0/−1 subspace uses only one component of the +1/−1 subspaces, which couples with the ^{13}C spin bath, the Ramsey coherence time T_{2}* should be double of the geometric qubit. However, the geometric qubit should surpasses the dynamical qubit with the multipulse echo^{17,31} even in the absence of magnetic field, as previously demonstrated in the presence of magnetic field^{32}. Since the dynamical Hahn echo cannot inverse the +1/−1 subspace, it cannot reverse time to recover the original state even in the absence of magnetic field. In contrast, the developed geometrical qubit defined in the +1/−1 subspace is spaceinversed by the geometrical echo and thus timereversed to decouple the spin bath.
We demonstrated the geometric spin echo of a degenerate geometric spin qubit via the ancillary state in a diamond NV centre. The geometric spin echo recovered the coherence imprinted in the degenerate subspace after 140 times the freeinduction decay time. The theoretical analysis indicates that the geometric spin qubit is three dimensionally protected against decoherence by the axial and transverse zerofield splittings with the help of timereversal, leaving decoherence due to dimer ^{13}C nuclear spins under a zero magnetic field. The purely geometric spin qubit is not only robust against noise caused by the spin bath but also robust against control error, and thus is suitable for a memory qubit used in quantum information and quantum sensing of magnetic, electric or strain fields for biomedical imaging.
Methods
Experimental setup
We used for the experiments a native NV centre in typeIIa highpressure hightemperature grown bulk diamond with a 〈001〉 crystal orientation (from Sumitomo Electric) without any irradiation or annealing. This diamond has NV centres (∼10^{12} cm^{−3}) and nitrogen impurities called P1 centres (<1 p.p.m.), leading to relatively higher density than a chemical vapour deposition grown diamond. A negatively charged NV centre located at ∼30 μm below the surface was found using a confocal laser microscope. A 25 μm copper wire mechanically attached to the surface of the diamond was used to apply a microwave for the ODMR measurement. An external magnetic field at an angle of 70° to the NV axis was applied to compensate the geomagnetic field of ∼0.045 mT using a permanent magnet. Careful orientation of the magnet was conducted with monitoring of the ODMR spectrum within 0.1 MHz. The Rabi oscillation and Ramsey interference were also used to finetune the field. The NV centre used in the experiment showed no hyperfine splitting caused by ^{13}C nuclear spins exceeding 0.1 MHz. All experiments were performed at room temperature.
Pulse sequences
The pulse sequences used in the demonstrations are summarized in Fig. 1d. Green light irradiation for 3 μs initializes the electron system into the ancillary state , which is followed by microwave pulses resonant to the zerofield splitting D with pulse patterns depending on the experiment. The Rabi oscillation between the bright state and the ancillary state was first observed to determine the π pulse width. The Ramsey interference was then observed to confirm the coherence between logical qubit basis states and by letting those superposition states revolve between and during the time between the two π pulses, instead of two π/2 pulses, as is used for the conventional Ramsey interference. Finally, we demonstrated the geometric spin echo by applying a 2π pulse in the middle of the free precession, instead of a π pulse as is used for the conventional Hahn echo. Despite the differences in the scheme, the random phase shift caused by the spin bath rephased back into the initial state as is schematically shown in the inset of Fig. 1d. The photon counts during the first 300 ns normalized by those during the last 2 μs of the 3μsgreen laser irradiation for the next initialization were used to measure the population in the 0〉 state. All the pulse sequences and photon counts were managed by an FPGAbased control system developed by NEC communications.
Calculation model
For the calculation of the magnetic field dependence of T_{2} echo time under a zero magnetic field, we neglected the T_{1} relaxation time since it is sufficiently longer than T_{2}. The decoherence is therefore dominated by the effects of single ^{13}C nuclear spins and dimers (nearestneighbour nuclear spin pair). Because of the large discrepancy in the Zeeman energy between the electron spin and the bath spins, we neglected the electron spin bit flip induced by the bath spins and attributed the coherence of the electron spin to that of the bath spins^{27,29},
where U^{(}^{)} is the time evolution operator depending the electron spin state and ρ_{N} is the spin bath state operator; at the hightemperature limit, (N: the number of bath spins). We considered only single and dimer ^{13}C nuclear spins as bath spins and neglected the interaction between bath spins^{28}. The electron spin echo signal could thus be factorized into individual bath spins as follows:
where S_{single,j}(2τ) is the jth single ^{13}C nuclear spin contribution and S_{dimer,k}(2τ) is the kth dimer ^{13}C nuclear spin contribution.
Electron spin decoherence
The dipole–dipole interaction between i spin and j spin is defined as
where μ_{0} is the vacuum permeability, γ_{i}(γ_{j}) is the gyromagnetic ratio of the i (j) spin (electron spin: γ_{e}=−1.76 × 10^{11} rad s^{−1} T^{−1}, ^{13}C nuclear spin: γ_{c}=6.73 × 10^{7} rad s^{−1} T^{−1}), S_{i} (S_{j}) is the spin operator of the i (j) spin and r_{i j} is the displacement of the i spin from the j spin. In the following, we describe S (I_{j}) as a spin1 operator of the electron spin (spin1/2 operator of jth ^{13}C nuclear spin). Hyperfine interaction conditioned by the electron spin eigenstates of the Hamiltonian in equation (1) can be represented as
where is the electron spin hyperfine field depending on the electron spin state . Then, we can define the effective magnetic field, Hamiltonian and time evolution operator depending on the electron spin state as
The echo signal given by the single jth ^{13}C spin is^{33}
These equations indicate that a single nuclear spin does not decohere the electron spin under a zero magnetic field after the spin echo, since the time evolution operators depending on the electron spin state are compatible, while it does decohere the electron spin under a nonzero magnetic field. On the other hand, the effective magnetic field, Hamiltonian and time evolution operator of the kth dimer are
where I_{k0}, I_{k1} are 0th, 1st ^{13}C spins consisting the dimer and we suppose that the effective magnetic field is applied equally to each nuclear spin. The echo signal given by the kth dimer is
The spin bath configuration is generated by randomly placing ^{13}C isotopes with natural abundance of 1.1% at a distance within 4 nm of the vacancy electron (Supplementary Fig. 2). T_{2} is determined by fitting with .
Transverse zerofield splitting
If we neglect the transverse magnetic field for simplicity, the Hamiltonian in equation (1) can be rewritten as + thus generating the following eigenenergies depending on the nitrogen nuclear spin states m_{I}=0, ±1
and eigenstates
where , are the polar and azimuth angles of the Bloch sphere spanned by ,
As the z component of the energy splitting decreases compared with the transverse zerofield splitting , where E_{x} (E_{y}) is x (y) component of the energy splitting, the m_{S}=±1 states couple strongly and finally become completely coupled states . The transverse zerofield splitting under the condition thus decouples the interaction between the electron spin and bath spins to suppress the decoherence effect by decreasing the electron spin hyperfine field . This protection effect explains the enhancement seen in Fig. 3b around 0 and 0.075 mT, where the nitrogen hyperfine field cancels out the z component of the external magnetic field on the electron spin. The enhancement becomes prominent by initializing the nitrogen nuclear spin state to m_{I}=0 state under a zero magnetic field, at which point the electron spin echo coherence time T_{2} drastically increase.
Data availability
The data that support the findings of this study are available from the corresponding author upon request.
Additional information
How to cite this article: Sekiguchi, Y. et al. Geometric spin echo under zero field. Nat. Commun. 7:11668 doi: 10.1038/ncomms11668 (2016).
References
 1.
Balasubramanian, G. et al. Ultralong spin coherence time in isotopically engineered diamond. Nat. Mater. 8, 383–387 (2009).
 2.
Ryan, C. A., Hodges, J. S. & Cory, D. G. Robust decoupling techniques to extend quantum coherence in diamond. Phys. Rev. Lett. 105, 200402 (2010).
 3.
Naydenov, B. et al. Dynamical decoupling of a singleelectron spin at room temperature. Phys. Rev. B 83, 081201 (2011).
 4.
BarGill, N., Pham, L. M., Jarmola, A., Budker, D. & Walsworth, R. L. Solidstate electronic spin coherence time approaching one second. Nat. Commun. 4, 1743 (2013).
 5.
Neumann, P. et al. Multipartite entanglement among single spins in diamond. Science 320, 1326–1329 (2008).
 6.
Pfaff, W. et al. Demonstration of entanglementbymeasurement of solidstate qubits. Nat. Phys. 9, 29–33 (2013).
 7.
Bernien, H. et al. Heralded entanglement between solidstate qubits separated by three metres. Nature 497, 86–90 (2013).
 8.
Pfaff, W. et al. Unconditional quantum teleportation between distant solidstate quantum bits. Science 345, 532–535 (2014).
 9.
Maze, J. R. et al. Properties of nitrogenvacancy centers in diamond: the group theoretic approach. New J. Phys. 13, 025025 (2011).
 10.
Zu, C. et al. Experimental realization of universal geometric quantum gates with solidstate spins. Nature 514, 72–75 (2014).
 11.
ArroyoCamejo, S., Lazariev, A., Hell, S. W. & Balasubramanian, G. Room temperature highfidelity holonomic singlequbit gate on a solidstate spin. Nat. Commun. 5, 4870 (2014).
 12.
Kosaka, H. et al. Coherent transfer of light polarization to electron spins in a semiconductor. Phys. Rev. Lett. 100, 096602 (2008).
 13.
Kosaka, H. et al. Spin state tomography of optically injected electrons in a semiconductor. Nature 457, 702–705 (2009).
 14.
Togan, E. et al. Quantum entanglement between an optical photon and a solidstate spin qubit. Nature 446, 730–734 (2010).
 15.
Kosaka, H. & Niikura, N. Entangled absorption of a single photon with a single spin in diamond. Phys. Rev. Lett. 114, 053603 (2015).
 16.
London, P., Balasubramanian, P., Naydenov, B., McGuinness, L. P. & Jelezko, F. Strong driving of a single spin using arbitrarily polarized fields. Phys. Rev. A 90, 012302 (2014).
 17.
Morton, J. J. L. et al. Bang–bang control of fullerene qubits using ultrafast phase gates. Nat. Phys. 2, 40–43 (2006).
 18.
Duan, L. M., Cirac, J. I. & Zoller, P. Geometric manipulation of trapped ions for quantum computation. Science 292, 1695–1697 (2001).
 19.
Berry, M. V. Quantal phasefactors accompanying adiabatic changes. Proc. R. Soc. Lond. A 392, 45–57 (1984).
 20.
Zanardi, P. & Rasetti, M. Holonomic quantum computation. Phys. Lett. A 264, 94–99 (1999).
 21.
Falci, G., Fazio, R., Palma, G. M., Siewert, J. & Vedral, V. Detection of geometric phases in superconducting nanocircuits. Nature 407, 355–358 (2000).
 22.
Solinas, P., Zanardi, P., Zanghi, N. & Rossi, F. Holonomic quantum gates: a semiconductorbased implementation. Phys. Rev. A 67, 062315 (2003).
 23.
Johansson, M. et al. Robustness of nonadiabatic holonomic gates. Phys. Rev. A 86, 062322 (2012).
 24.
Jones, J. A., Vedral, V., Ekert, A. & Castagnoli, G. Geometric quantum computation using nuclear magnetic resonance. Nature 403, 869–871 (1999).
 25.
Feng, G., Xu, G. & Long, G. Experimental realization of nonadiabatic holonomic quantum computation. Phys. Rev. Lett. 110, 190501 (2013).
 26.
Abdumalikov, A. A. et al. Experimental realization of nonAbelian nonadiabatic geometric gates. Nature 496, 482–485 (2013).
 27.
Maze, J. R., Taylor, J. M. & Lukin, M. D. Electron spin decoherence of single nitrogenvacancy defects in diamond. Phys. Rev. B 78, 094303 (2008).
 28.
Yang, W. & Liu, R. B. Quantum manybody theory of qubit decoherence in a finitesize spin bath. Phys. Rev. B 78, 085315 (2008).
 29.
Zhao, N., Ho, S. W. & Liu, R. B. Decoherence and dynamical decoupling control of nitrogen vacancy center electron spins in nuclear spin baths. Phys. Rev. B 85, 115303 (2012).
 30.
Dolde, F. et al. Electricfield sensing using single diamond spins. Nat. Phys. 7, 459–463 (2011).
 31.
de Lange, G., Wang, Z. H., Ristè, D., Dobrovitski, V. V. & Hanson, R. Universal dynamical decoupling of a single solidstate spin from a spin bath. Science 330, 60–63 (2010).
 32.
Huang, P. et al. Observation of an anomalous decoherence effect in a quantum bath at room temperature. Nat. Commun. 2, 570 (2011).
 33.
Childress, L. et al. Coherent dynamics of coupled electron and nuclear spin qubits in diamond. Science 314, 281–285 (2006).
Acknowledgements
We thank Yuichiro Matsuzaki, Fedor Jelezko, Burkhard Scharfenberger, Kae Nemoto, William Munro, Norikazu Mizuochi and Jöerg Wrachtrup for their discussions and experimental help. This work was supported by the NICT Quantum Repeater Project, by the FIRST Quantum Information Project, and by a GrantinAid for Scientific Research (A)JSPS (No. 24244044).
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Affiliations
Department of Physics, Electrical and Computer Engineering, Graduate School of Engineering, Yokohama National University, 795 Tokiwadai, Hodogaya, Yokohama 2408501, Japan
 Yuhei Sekiguchi
 , Yusuke Komura
 , Shota Mishima
 , Touta Tanaka
 , Naeko Niikura
 & Hideo Kosaka
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Contributions
The experiment was designed and analysed by Y.S., Y.K. and H.K. Measurements were made by Y.S. and Y.K. S.M., T.T. and N.N. supported the experiments in technical matters. H.K. supervised the experiments. Y.S., Y.K. and H.K. wrote the paper.
Competing interests
The authors declare no competing financial interests.
Corresponding author
Correspondence to Hideo Kosaka.
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Further reading

1.
Optical holonomic single quantum gates with a geometric spin under a zero field
Nature Photonics (2017)
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