Article | Open | Published:

# Nanoscale zero-field electron spin resonance spectroscopy

## Abstract

Electron spin resonance (ESR) spectroscopy has broad applications in physics, chemistry, and biology. As a complementary tool, zero-field ESR (ZF-ESR) spectroscopy has been proposed for decades and shown its own benefits for investigating the electron fine and hyperfine interaction. However, the ZF-ESR method has been rarely used due to the low sensitivity and the requirement of much larger samples than conventional ESR. In this work, we present a method for deploying ZF-ESR spectroscopy at the nanoscale by using a highly sensitive quantum sensor, the nitrogen vacancy center in diamond. We also measure the nanoscale ZF-ESR spectrum of a few P1 centers in diamond, and show that the hyperfine coupling constant can be directly extracted from the spectrum. This method opens the door to practical applications of ZF-ESR spectroscopy, such as investigation of the structure and polarity information in spin-modified organic and biological systems.

## Introduction

Electron spin resonance (ESR) spectroscopy is a method for studying paramagnetic targets, including metal complexes and organic radicals. Combining with site-directed spin-labeling of radicals, ESR has been widely used to study basic molecular mechanisms in biological systems1, such as structure2, dynamics3, and polarity4. This information is derived from the electron fine and hyperfine interaction, which can be obtained from the ESR spectra with accuracy limited by the inhomogeneous line broadening. The line broadening of powder spectra, induced by the magnetic inequivalence of otherwise-identical spins, can be partly removed in high-field ESR (HF-ESR) experiment5. A complete removal can be achieved by zero-field ESR (ZF-ESR) spectroscopy6,7,8,9 because the energy levels of a spin system are no longer orientation dependent in the absence of a Zeeman term. Although the ZF-ESR spectroscopy provides a straightforward method for investigating the intrinsic interactions, it has rare applications due to the much lower sensitivity compared with the conventional ESR (henceforth, ESR refers to non-zero field ESR).

Nitrogen vacancy (NV) centers in diamond can be used as magnetic quantum sensors to significantly improve the sensitivity10,11,12,13. NV center-based ESR has been demonstrated using both double electron–electron resonance (DEER)14,15,16 and cross-polarization methods17,18, and detection of single electron spins has been realized19,20. However, these methods cannot be directly used in zero field because of the complication of manipulating target spins in zero field.

Here we propose a different method, which does not require any manipulation of target spins, and allows for detecting nanoscale ZF-ESR signals. It is achieved by precisely tuning the energy levels of NV centers in dressed states to be resonant with target spins. We also demonstrate it by detecting the ZF-ESR spectrum of a few P1 centers residing at a distance of less than 15 nanometers from the NV center. By analyzing the resonance lines, the intrinsic interactions, such as hyperfine interaction, can be directly resolved. Moreover, we show that the nanoscale ZF-ESR can perform significantly better than nanoscale ESR without loss of sensitivity.

## Results

### Scheme of zero-field detection using an NV spin

The basic essence of our method is shown in Fig. 1a, where the sensors are shallow NV centers embedded in a bulk diamond. The diamond is adhered on a coplanar waveguide, and observed by a home-built confocal microscope from the other side. As illustrated in Fig. 1b, the NV centers are surrounded by a spin mixture consisting of target spins and background spins. The target spins can be either defects inside the diamond or paramagnetic targets on the diamond surface. The background spins are dangling bonds on the diamond surface. The NV center is a kind of color defect in diamond consisting of a substitutional nitrogen atom and an adjacent vacancy (see Fig. 1c). The electrons around the defect form an effective electron spin with a spin triplet ground state (S = 1) and a zero-field splitting of D = 2π × 2.87 GHz21. The NV electron spin can be polarized into the $$\left| {m_{\mathrm{s}} = 0} \right\rangle$$ state ($$\left| 0 \right\rangle$$, henceforth) by 532 nm laser excitation. The photoluminescence (PL) rate of NV center is state-dependent, i.e., $$\left| 0 \right\rangle$$ is “brighter” than $$\left| { \pm 1} \right\rangle$$, then the populations of the states can be directly read out by the photoluminescence rate. Furthermore, the spin transition between $$\left| 0 \right\rangle$$ and $$\left| { \pm 1} \right\rangle$$ can be driven by the microwave. As shown in Fig. 1d, under resonant microwave (B1 cos ft, f = D) radiation, the NV electron spin can be driven to the dressed states, which are

$$\begin{array}{l}\left| { - 1} \right\rangle _{\mathrm{d}} = \frac{1}{2}\left| 1 \right\rangle - \frac{1}{{\sqrt 2 }}\left| 0 \right\rangle + \frac{1}{2}\left| { - 1} \right\rangle ,\\ \left| 0 \right\rangle _{\mathrm{d}} = - \frac{1}{{\sqrt 2 }}\left| 1 \right\rangle + \frac{1}{{\sqrt 2 }}\left| { - 1} \right\rangle ,\\ \left| 1 \right\rangle _{\mathrm{d}} = \frac{1}{2}\left| 1 \right\rangle + \frac{1}{{\sqrt 2 }}\left| 0 \right\rangle + \frac{1}{2}\left| { - 1} \right\rangle ,\end{array}$$
(1)

in the rotating reference frame with eigenenergies −Ω/2, 0, and Ω/2, respectively. Here, Ω is the driving power valued by the corresponding Rabi frequency with Ω = γNVB1, proportional to the perpendicular amplitude of the driving microwave, where γNV = −2π × 2.803 MHz/G is the gyromagnetic ratio of the NV electron spin. Similar to the Hartmann–Hahn double resonance22,23, the dipole–dipole interaction between the NV center and the target spins will induce a flip-flop process at the resonance condition

$${\mathrm{\Omega }} = 2{\mathrm{\Delta }}\omega _{ij},$$
(2)

where Δω ij  = ω j  − ω i (i < j) is the energy level splitting of the target spins corresponding to an allowed magnetic dipole transition. If the NV center is initially polarized to one of the dressed states given by Eq. (1), the polarization will be transferred from the NV center to the target spins, then the populations of dressed states will change. Therefore, a resonance spectrum of the target spins can be measured by sweeping the driving power and measuring the populations of the dressed states.

In zero magnetic field, all the Zeeman terms vanish and the energy level structure of the target spins is determined solely by the intrinsic spin–spin interactions. To see how these interactions can be resolved by ZF-ESR, we take a free radical with hyperfine interaction between the electron spin S and the nuclear spin I as an example. For clarity, here we deal with S = 1/2 and I = 1/2 (for I = 1 nuclei, see Supplementary Note 5). The Hamiltonian of the target spin can be written as24

$$H_0 = {\bf{S}} \cdot {\Bbb A} \cdot {\bf{I}},$$
(3)

where $${\Bbb A}$$ is the hyperfine tensor, which is diagonal

$${\Bbb A} = \left( {\begin{array}{*{20}{c}} {A_{xx}} & {} & {} \\ {} & {A_{yy}} & {} \\ {} & {} & {A_{zz}} \end{array}} \right)$$
(4)

in the principal axis frame. The eigenstates of Eq. (3) are

$$\begin{array}{l}\left| {\phi _1} \right\rangle = \frac{1}{{\sqrt 2 }}\left( {\left| { \uparrow \downarrow } \right\rangle - \left| { \downarrow \uparrow } \right\rangle } \right),\\ \left| {\phi _2} \right\rangle = \frac{1}{{\sqrt 2 }}\left( {\left| { \uparrow \downarrow } \right\rangle + \left| { \downarrow \uparrow } \right\rangle } \right),\\ \left| {\phi _3} \right\rangle = \frac{1}{{\sqrt 2 }}\left( {\left| { \uparrow \uparrow } \right\rangle - \left| { \downarrow \downarrow } \right\rangle } \right),\\ \left| {\phi _4} \right\rangle = \frac{1}{{\sqrt 2 }}\left( {\left| { \uparrow \uparrow } \right\rangle + \left| { \downarrow \downarrow } \right\rangle } \right),\end{array}$$
(5)

where $$\left| \uparrow \right\rangle$$ and $$\left| \downarrow \right\rangle$$ denote spin-up and spin-down, respectively, with the electron spin on the left and the nuclear spin on the right. The corresponding eigenenergies are

$$\begin{array}{l}\omega _1 = \frac{1}{4}\left( { - A_{xx} - A_{yy} - A_{zz}} \right),\\ \omega _2 = \frac{1}{4}\left( {A_{xx} + A_{yy} - A_{zz}} \right),\\ \omega _3 = \frac{1}{4}\left( { - A_{xx} + A_{yy} + A_{zz}} \right),\\ \omega _4 = \frac{1}{4}\left( {A_{xx} - A_{yy} + A_{zz}} \right).\end{array}$$
(6)

Six allowed magnetic dipole transitions between these states are expected with frequencies

$$\begin{array}{*{20}{l}} {{\mathrm{\Delta }}\omega _{12} = \frac{1}{2}\left| {A_{xx} + A_{yy}} \right|,{\mathrm{\Delta }}\omega _{34} = \frac{1}{2}\left| {A_{xx} - A_{yy}} \right|,} \hfill \\ {{\mathrm{\Delta }}\omega _{13} = \frac{1}{2}\left| {A_{yy} + A_{zz}} \right|,{\mathrm{\Delta }}\omega _{24} = \frac{1}{2}\left| {A_{yy} - A_{zz}} \right|,} \hfill \\ {{\mathrm{\Delta }}\omega _{14} = \frac{1}{2}\left| {A_{xx} + A_{zz}} \right|,{\mathrm{\Delta }}\omega _{23} = \frac{1}{2}\left| {A_{xx} - A_{zz}} \right|.} \hfill \end{array}$$
(7)

Note that a rotational transformation does not change the eigenenergies, which means that these transition frequencies are independent of the orientation of the radicals, while the transition speed determined by the dipole–dipole interaction between the NV center and the radicals is orientation-dependent. A detailed discussion can be found in Supplementary Note 1.

### Experimental demonstration

We perform the measurement on a similar electron-nuclear system named a P1 center, which is another kind of defect in diamond consisting of only a substitutional nitrogen atom. For a 15N P1 center, the principal values of the hyperfine tensor are A xx  = A yy  = A = 114 MHz and A zz  = 159.9 MHz25. Due to the Jahn–Teller effect, one of the nitrogen–carbon bonds is distorted, and the orientation of a P1 center can change between the four kinds of N–C bonds26. The NV and P1 centers are generated by ion implantation. To make the P1 centers close enough to the NV centers, the diamond we used is implanted with high dose of nitrogen ions (see “Methods”). So the experiment is performed on an ensemble of NV centers with each NV center surrounded by dozens of P1 centers. As demonstrated by Hall et al.18, the NV center is a highly local sensor. Although ensembles of NV and P1 centers are involved, the response of each NV center is dominated by only those P1 centers residing in its nanoscale detection area (a quantitative discussion is given below). Therefore, each NV center is an isolated sensor, and the detected ZF-ESR spectrum is the average spectrum of P1 centers in each nanoscale region. Since the resonance frequencies of different P1 centers are the same, using ensembles of NV centers can speed up the measurement.

Unlike the frequency-sweeping method14,15,16,19,20, where the microwave frequency can be easily tuned, the microwave power is limited by the microwave amplifier and the transform efficiency of the waveguide. Here, by using a proper designed coplanar waveguide, a Rabi frequency up to ~400 MHz was realized (see Fig. 2a, c), enough to capture all the interaction information of P1 centers. We note that by further employing a high-power microwave amplifier and shaped pulses, Rabi frequencies ~1 GHz are possible27, which is theoretically limited by the zero-field splitting of NV centers. Then, this method is applicable to more high-spin paramagnetic targets. On the other hand, the lower limit of the Rabi frequency is bounded by the dephasing time of NV centers. The NV centers have four kinds of directions, so the B1, on different NV sites may be different, which induces an extra sine modulation on the Rabi oscillation. Comparing with the Rabi oscillation, where the NV state is rotating between $$\left| 0 \right\rangle$$ and $$\left| { \pm 1} \right\rangle$$, the NV state is locked in $$\left| { - 1} \right\rangle _{\mathrm{d}}$$ by applying a π/2 pulse with 90° phase difference before the continuous driving (see “Methods” and Fig. 2b). The experimental result in Fig. 2d shows that the NV state is successfully locked with a relaxation time of T1ρ = 70 ± 2 μs, which is much longer than the dephasing time of $$T_2^ \ast \sim 0.1$$ μs.

The ZF-ESR spectrum is obtained by sweeping the driving power while fixing the driving length τ = 10 μs, as illustrated in Fig. 3a. Since the hyperfine tensor $${\Bbb A}$$ of P1 centers is cylindrically symmetrical, the eigenstate $$\left| {\phi _3} \right\rangle$$ and $$\left| {\phi _4} \right\rangle$$ are degenerate, thus only three magnetic dipole transitions are observable (see Fig. 3b). Figure 3c gives the measured spectrum with three characteristic peaks at 44.0 ± 3.6, 221.7 ± 3.4, and 270.8 ± 4.8 MHz, where the error bars are given by half the linewidths of the Gaussian peaks. It seems like there are other peaks at ~80 and ~130 MHz. The reason is unknown yet. A possible source of these extra signals is other kinds of defects, due to the numerous electron spin defects in diamond28. As the spin-locking relaxation time T1ρ depends on the driving power Ω, the baseline of the original ZF-ESR spectrum is uneven (Supplementary Note 3), which has been calibrated to unity as shown in Fig. 3c. Combining with Eqs. (2) and (7), the principal values of the hyperfine tensor can be directly obtained from any two peaks or a least-squares fitting of all the three peaks. The least-squares fitting gives $$A_ \bot ^{{\mathrm{exp}}}$$ = 110.7 ± 3.5 MHz and $$A_{zz}^{{\mathrm{exp}}}$$ = 155.0 ± 7.1 MHz, consistent with the hyperfine coupling of 15N P1 center. We have also measured the ZF-ESR spectrum of 14N P1 center, which can be found in Supplementary Note 5.

The energy level shifts induced by the environmental fluctuations on either the NV center or the P1 center will destroy the energy exchange between them, which acts to broaden the resonance frequencies, as characterized by the transverse spin relaxation rate, Γtot = ΓNV + ΓP1. The transverse spin relaxation of the NV center can be significantly suppressed by continuously driving29, so $${\mathrm{\Gamma }}_{{\mathrm{tot}}} \approx {\mathrm{\Gamma }}_{{\mathrm{P1}}} = 1{\mathrm{/}}T_{2,{\mathrm{P1}}}^ \ast$$. The dephasing time of the P1 centers can be estimated by the dephasing time of the NV center, which is ~0.1 μs, because of the similar environment of the NV and P1 centers. Thus, the linewidth induced by the dephasing is $${\mathrm{\Delta \Omega }}\sim 1{\mathrm{/}}\left( {\pi T_{2,{\mathrm{P1}}}^ \ast } \right)$$ ~ 3.2 MHz17, not enough to explain the observed linewidth of 7 ~ 10 MHz. Besides, the fluctuations of the driving power will also induce the broadening of zero-field lines. It was recorded and calibrated during the measurement with fluctuation <0.5% (Supplementary Note 4). Moreover, the residual static magnetic field (mainly contributed by the geomagnetic field) will induce line splitting of ~2.3 MHz (Supplementary Note 4), which will behave as line broadening if the line splitting is smaller than the linewidth. The residual field can be further avoided by placing the setup in a mu-metal box or actively compensating with an electromagnetic field.

To confirm that the detected spectrum is indeed dominated by the P1 centers in a nanoscale detection area, we have calculated the signal induced by all the P1 centers residing at a distance of >15 nm from the NV center, which is ≤0.29% (see “Methods”). While the signal contrast in Fig. 3c is ~3%, indicates more than 90% of the signal is attributable to the P1 centers residing in the detection area with radius of 15 nm. The mean number of P1 centers in this detection area is ~4. Note that it is a conservative estimate, as the peaks in Fig. 3c are broadened by some additional effects which will lower the signal contrast.

### Comparison to nanoscale ESR

In some practical nanoscale applications, such as detection of nitroxide radicals dispersed on the diamond surface, the NV center-based ZF-ESR can outperform NV center-based ESR (here we take DEER as an example) for several reasons, including the following. First, the ZF-ESR method, which does not require an external magnet or manipulation of the target spins (see Fig. 4a, b), will be easily used. Second, unlike the inner P1 centers, which are restricted by the diamond lattice and have only four orientations, the external nitroxides are much more disordered and can be oriented in any direction16,20. The simulated spectra with different orientations of nitroxide are given in Fig. 4c, d. Since the DEER spectrum is orientation-dependent, the peaks will be averaged if differently oriented nitroxides are included. For conventional induction-based ESR, the statistical average of the orientations over a large ensembles of spins induces an inhomogeneously broadened powder spectrum, where the hyperfine values can still be extracted even with limited accuracy. But for nanoscale ESR, the detected spins are much fewer (~101), then the average spectrum (see Fig. 4e) still has a certain randomness. Without prior knowledge of the orientations of each nitroxide, extraction of the hyperfine values will be nearly impossible. However, for the ZF-ESR spectrum, different orientations will lead to different peak intensities rather than peak positions, so the characteristic peaks remain clear in the ZF-ESR spectrum (see Fig. 4f) all the time. Third, there exists a paramagnetic background, which consists of dangling bonds on the diamond surface with g factor similar to free radicals30,31,32. Due to the dense distribution and the short correlation time30,33,34, the background spins always behave as a broad central peak in the DEER spectrum (see Fig. 4e and Supplementary Note 2), which can be hardly distinguished from the nitroxides. While in zero field, the background peak will move to the zero frequency and only a characterless low-frequency signal can be observed (see Fig. 4f and Supplementary Note 2), thus the fingerprint-like ZF-ESR signal of target spins can be naturally distinguished.

On the other hand, unlike the conventional induction-based ESR, where the signal intensity is proportional to the polarization of the electron spins (i.e., the magnetic field), the signal of NV center-based ESR is induced by the statistically polarized electron spins. So, the sensitivity of this nanoscale ESR does not depend on the magnetic field. Specifically, the nanoscale detection is based on dipole–dipole coupling between the probe and the target and limited by the coherence properties of the probe. For DEER measurement, only zz coupling contributes to the signal, and the sensitivity is limited by the T2 of the NV center12. For our ZF-ESR measurement, all the zx, zy, and zz couplings contribute to the signal (detail in Supplementary Note 1), and the sensitivity is limited by the T1ρ of the NV center, which is usually much longer than T2. Therefore, the sensitivity of our nanoscale ZF-ESR is comparable with and even potentially better than the nanoscale ESR.

## Discussion

In conclusion, we have presented a method for measuring the ZF-ESR spectrum of nanoscale paramagnetic samples, via continuously tuning the energy levels of NV centers in dressed states. The significant improvement of the sensitivity of ZF-ESR removes the biggest obstacle to applications of ZF-ESR spectroscopy. The nanoscale ZF-ESR can also outperform the previous nanoscale ESR. The method is demonstrated by successful measurement of the ZF-ESR spectrum of a few P1 centers at the nanoscale. Unlike the conventional ESR spectrum which is complicated due to the orientation-dependent resonance frequencies, our method of measurement in zero field can unambiguously give a characteristic resonance spectrum determined solely by the intrinsic interactions of the target spins, and thus the interaction structure can be directly resolved. It was found that the hyperfine interaction has a strong relation to the polarity profiles and hydrogen bonding effects of molecules4, so this method can be used further to analyze the micro-environment information of molecules. Although this work is focused on the electron–nuclear hyperfine interaction, we note that the key element of the technique is the direct measurement of the energy level structure of paramagnetic targets, regardless of the form of interaction. This technique can also be used to analyze the electron–electron spin interaction, which contains the structure information of molecules2.

## Methods

### Experimental setup

The setup is based on a home-built confocal microscopy. A temperature-stabilized diode laser (CNI MGL-III-532) is used for the polarization and readout of the NV centers. The photoluminescence is detected by an Avalanche photodiode (Perkin Elmer SPCM-AQRH-14) through a ×60, 0.7 NA objective (Olympus LUCPLFLN). The driving microwave is generated by an arbitrary waveform generator (Agilent M8190a) and amplified by a microwave amplifier (Mini-circuits ZHL-16W-43+). The diamond is obtained commercially, 100-oriented, and electronic-grade with a thickness of 500 μm. The NV and P1 centers were created by implantation of 5 keV 15N+ ions with dose of 5.5 × 1011 cm−2. The mean spacing of N atoms is 13.5 nm. The production efficiency of NV centers is ~1%, and then the mean spacing of NV centers is ~135 nm. The mean depth of N atom is estimated to be 8 ± 3.2 nm by SRIM, while the actual depth may be larger35.

### Detection area

Since the NV and P1 centers are created by the implantation of N+ ions, we suppose both of them are located in a thin layer and only the transverse distance is considered. It is reasonable when the transverse distance is much larger than the longitudinal straggling. Here, we consider the sum of the signal contributed by all the P1 centers out of the detection area, which can be given by (see Supplementary Note 1)

$$\begin{array}{*{20}{l}} {S^{{\mathrm{sum}}}\left( {r > r_0} \right)} \hfill & = \hfill & {\mathop {\sum}\limits_{r > r_0} \frac{{C_0^2\left\langle {\eta ^2} \right\rangle \tau }}{{8{\mathrm{\Gamma }}_{{\mathrm{P1}}}r^6}}} \hfill \\ {} \hfill & = \hfill & {{\int}_{r_0}^\infty \frac{{C_0^2\left\langle {\eta ^2} \right\rangle \tau }}{{8{\mathrm{\Gamma }}_{{\mathrm{P1}}}r^6}} \cdot \sigma \cdot 2\pi r\mathrm{d}r} \hfill \\ {} \hfill & = \hfill & {\frac{{\pi \sigma C_0^2\left\langle {\eta ^2} \right\rangle \tau }}{{16{\mathrm{\Gamma }}_{{\mathrm{P1}}}r_0^4}},} \hfill \end{array}$$
(8)

where σ = 5.5 × 1011 cm−2 is the area density of P1 centers, C0 = 2π × 52 MHz nm3 is the dipolar coupling constant, η is the coefficient of dipole–dipole coupling depending on both the direction of the spatial separation r and the P1 center. After averaging over all the possible directions, $$\left\langle {\eta ^2} \right\rangle$$ is calculated to be 5/4 or 3/4 corresponding to the left/right or middle peak in Fig. 3c. Other parameters in this experiment are ΓP1 = 10 MHz and τ = 10 μs. Hence, the sum of signals contributed by those P1 centers out of the detection area decreases dramatically with the radius of the area. For example, if r0 = 15 nm, then Ssum can be calculated to be 0.29%, 0.17%, and 0.29% for the left, middle, and right peaks, respectively.

### Spin locking in zero field

The Hamiltonian of NV center in zero magnetic field is

$$H_0 = DS_z^2,$$
(9)

where S(S = 1) is the NV electron spin operators, D = 2π × 2.87 GHz is the zero-field splitting. The NV center can be driven by the microwave of the form

$$H_1 = {\mathrm{\Omega }}{\kern 1pt} {\mathrm{cos}}\left( {ft + \phi } \right)S_x,$$
(10)

where Ω, f, and ϕ are the power, frequency, and phase of the microwave, respectively, f = D in the resonance condition. In rotating reference frame, the Hamiltonian becomes

$$\begin{array}{*{20}{l}} {H^{{\mathrm{rot}}}} \hfill & = \hfill & {e^{iDS_z^2t}\left( {H_0 + H_1} \right)e^{ - iDS_z^2t} - DS_z^2} \hfill \\ {} \hfill & = \hfill & {\frac{{\mathrm{\Omega }}}{{2\sqrt 2 }}\left( {\begin{array}{*{20}{c}} 0 & {e^{ - i\phi }} & 0 \\ {e^{i\varphi }} & 0 & {e^{i\phi }} \\ 0 & {e^{ - i\phi }} & 0 \end{array}} \right),} \hfill \end{array}$$
(11)

where the high frequency items are ignored. By defining ϕ = 0, π/2, and −π/2 for x, y, and −y phase, respectively, we can write

$$\begin{array}{l}H_x^{{\mathrm{rot}}} = \frac{{\mathrm{\Omega }}}{2}S_x,\\ H_y^{{\mathrm{rot}}} = \frac{{\mathrm{\Omega }}}{2}S_{yy},\\ H_{ - y}^{{\mathrm{rot}}} = - \frac{{\mathrm{\Omega }}}{2}S_{yy}.\end{array}$$
(12)

Note here

$$S_{yy} = \frac{1}{{\sqrt 2 }}\left( {\begin{array}{*{20}{c}} 0 & { - i} & 0 \\ i & 0 & i \\ 0 & { - i} & 0 \end{array}} \right)$$
(13)

is slightly different from S y . The eigenstates and eigenenergies of $$H_x^{{\mathrm{rot}}}$$ can be directly calculated as given in the main text Eq. (1). The spin-locking sequence is performed as following:

First, the initial state of the NV center is polarized to $$\left| {\psi _0} \right\rangle = \left| 0 \right\rangle$$ by a laser pulse. Then, a y-phase π/2 pulse with power Ω0 and length tπ/2 = 1/(4Ω0) is applied and the NV state is prepared to

$$\begin{array}{*{20}{l}} {\left| {\psi _1} \right\rangle } \hfill & = \hfill & {e^{ - i2\pi H_y^{{\mathrm{rot}}}t_{\pi /2}}\left| {\psi _0} \right\rangle } \hfill \\ {} \hfill & = \hfill & {\frac{1}{2}\left| 1 \right\rangle - \frac{1}{{\sqrt 2 }}\left| 0 \right\rangle + \frac{1}{2}\left| { - 1} \right\rangle \equiv \left| { - 1} \right\rangle _{\mathrm{d}}.} \hfill \end{array}$$
(14)

Second, a x-phase pulse with power Ω and length τ is applied. Since $$\left| {\psi _1} \right\rangle$$ is an eigenstate of $$H_x^{{\mathrm{rot}}}$$, the state will be locked in $$\left| {\psi _1} \right\rangle$$. However, it can be transferred to other dressed states by T1ρ relaxation or coupling with nearby P1 centers. Supposing the transition probability is P, then the state becomes

$$\rho _2 = (1 - P)\left| { - 1} \right\rangle _{\mathrm{d}}\left\langle { - 1} \right| + P\left( {p_1\left| 0 \right\rangle _{\mathrm{d}}\left\langle 0 \right| + p_2\left| 1 \right\rangle _{\mathrm{d}}\left\langle 1 \right|} \right).$$
(15)

where p1 + p2 = 1.

Finally, a −y-phase π/2 pulse with power Ω0 and length tπ/2 = 1/(4Ω0) is applied. The state $$\left| { - 1} \right\rangle _{\mathrm{d}}$$ will be rotated back to $$\left| 0 \right\rangle$$, while $$\left| 0 \right\rangle _{\mathrm{d}}$$ remains unchanged and $$\left| 1 \right\rangle _{\mathrm{d}}$$ will be rotated to $$\left| 0 \right\rangle _{\mathrm{d}}$$. Therefore, the final state is

$$\rho _3 = (1 - P)\left| 0 \right\rangle \left\langle 0 \right| + P\left( {\left| 1 \right\rangle \left\langle 1 \right| - \left| 1 \right\rangle \left\langle { - 1} \right| - \left| { - 1} \right\rangle \left\langle 1 \right| + \left| { - 1} \right\rangle \left\langle { - 1} \right|} \right),$$
(16)

with the normalized photoluminescence of 1 − P.

### Data availability

Data supporting the findings of this study are available within the article and its Supplementary Information file, and from the corresponding authors on reasonable request.

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

## References

1. 1.

Borbat, P. P., Costa-Filho, A. J., Earle, K. A., Moscicki, J. K. & Freed, J. H. Electron spin resonance in studies of membranes and proteins. Science 291, 266–269 (2001).

2. 2.

Rabenstein, M. D. & Shin, Y. K. Determination of the distance between two spin labels attached to a macromolecule. Proc. Natl Acad. Sci. USA 92, 8239–8243 (1995).

3. 3.

Franck, J. M., Ding, Y., Stone, K., Qin, P. Z. & Han, S. Anomalously rapid hydration water diffusion dynamics near DNA surfaces. J. Am. Chem. Soc. 137, 12013–12023 (2015).

4. 4.

Kurad, D., Jeschke, G. & Marsh, D. Lipid membrane polarity profiles by high-field EPR. Biophys. J. 85, 1025–1033 (2003).

5. 5.

Smirnov, A. I. Electron Paramagnetic Resonance Vol. 18 (eds Gilbert, B. C., Davies, M. J. & Murphy, D. M.) 109–136 (The Royal Society of Chemistry, Cambridge, 2002).

6. 6.

Bogle, G. S., Symmons, H. F., Burgess, V. R. & Sierins, J. V. Paramagnetic resonance spectrometry at zero magnetic field. Proc. Phys. Soc. 77, 561–566 (1961).

7. 7.

Cole, T., Kushida, T. & Heller, H. C. Zero-field electron magnetic resonance in some inorganic and organic radicals. J. Phys. Chem. 38, 2915–2924 (1963).

8. 8.

Bramley, R. & Strach, S. J. Electron paramagnetic resonance spectroscopy at zero magnetic field. Chem. Rev. 83, 49–82 (1983).

9. 9.

Bramley, R. Variable-frequency electron paramagnetic resonance. Int. Rev. Phys. Chem. 5, 211–217 (1986).

10. 10.

Balasubramanian, G. et al. Nanoscale imaging magnetometry with diamond spins under ambient conditions. Nature 455, 648–651 (2008).

11. 11.

Maze, J. R. et al. Nanoscale magnetic sensing with an individual electronic spin in diamond. Nature 455, 644–647 (2008).

12. 12.

Taylor, J. M. et al. High-sensitivity diamond magnetometer with nanoscale resolution. Nat. Phys. 4, 810–816 (2008).

13. 13.

Degen, C. L., Reinhard, F. & Cappellaro, P. Quantum sensing. Rev. Mod. Phys. 89, 035002 (2017).

14. 14.

Grotz, B. et al. Sensing external spins with nitrogen-vacancy diamond. New J. Phys. 13, 055004 (2011).

15. 15.

Mamin, H. J., Sherwood, M. H. & Rugar, D. Detecting external electron spins using nitrogen-vacancy centers. Phys. Rev. B 86, 195422 (2012).

16. 16.

Schlipf, L. et al. A molecular quantum spin network controlled by a single qubit. Sci. Adv. 3, e1701116 (2017).

17. 17.

Belthangady, C. et al. Dressed-state resonant coupling between bright and dark spins in diamond. Phys. Rev. Lett. 110, 157601 (2013).

18. 18.

Hall, L. T. et al. Detection of nanoscale electron spin resonance spectra demonstrated using nitrogen-vacancy centre probes in diamond. Nat. Commun. 7, 10211 (2016).

19. 19.

Shi, F. et al. Quantum logic readout and cooling of a single dark electron spin. Phys. Rev. B 87, 195414 (2013).

20. 20.

Shi, F. et al. Single-protein spin resonance spectroscopy under ambient conditions. Science 347, 1135–1138 (2015).

21. 21.

Doherty, M. W. et al. The nitrogen-vacancy colour centre in diamond. Phys. Rep. 528, 1–45 (2013).

22. 22.

Hartmann, S. R. & Hahn, E. L. Nuclear double resonance in the rotating frame. Phys. Rev. 128, 2042–2053 (1962).

23. 23.

Henstra, A., Dirksen, P., Schmidt, J. & Wenckebach, W. Nuclear spin orientation via electron spin locking (novel). J. Magn. Reson. 77, 389–393 (1988).

24. 24.

McConnell, H. M., Thompson, D. D. & Fessenden, R. W. Hyperfine absorption spectrum of CH (COOH)2. Proc. Natl Acad. Sci. USA 45, 1600–1601 (1959).

25. 25.

Smith, W. V., Sorokin, P. P., Gelles, I. L. & Lasher, G. J. Electron-spin resonance of nitrogen donors in diamond. Phys. Rev. 115, 1546–1552 (1959).

26. 26.

Xiao, X. & Zhao, N. Proposal for observing dynamic Jahn-Teller effect by single solid-state defects. New J. Phys. 18, 103022 (2016).

27. 27.

Fuchs, G. D., Dobrovitski, V. V., Toyli, D. M., Heremans, F. J. & Awschalom, D. D. Gigahertz dynamics of a strongly driven single quantum spin. Science 326, 1520–1522 (2009).

28. 28.

Zaitsev, A. M. Optical Properties of Diamond (Springer, Berlin, 2001).

29. 29.

Xu, X. et al. Coherence-protected quantum gate by continuous dynamical decoupling in diamond. Phys. Rev. Lett. 109, 070502 (2012).

30. 30.

Grinolds, M. S. et al. Subnanometre resolution in three-dimensional magnetic resonance imaging of individual dark spins. Nat. Nanotechnol. 9, 279–284 (2014).

31. 31.

Sushkov, A. O. et al. Magnetic resonance detection of individual proton spins using quantum reporters. Phys. Rev. Lett. 113, 197601 (2014).

32. 32.

Kim, M. et al. Decoherence of near-surface nitrogen-vacancy centers due to electric field noise. Phys. Rev. Lett. 115, 087602 (2015).

33. 33.

Rosskopf, T. et al. Investigation of surface magnetic noise by shallow spins in diamond. Phys. Rev. Lett. 112, 147602 (2014).

34. 34.

Myers, B. A. et al. Probing surface noise with depth-calibrated spins in diamond. Phys. Rev. Lett. 113, 027602 (2014).

35. 35.

Lehtinen, O. et al. Molecular dynamics simulations of shallow nitrogen and silicon implantation into diamond. Phys. Rev. B 93, 035202 (2016).

## Acknowledgements

This work was supported by the 973 Program (Grants No. 2016YFA0502400 and 2013CB921800), the National Natural Science Foundation of China (Grants No. 11227901, 91636217, 11722544, 31470835, and 81788104), the CAS (Grants No. XDB01030400, QYZDY-SSW-SLH004, and YIPA2015370), the CEBioM, and the Fundamental Research Funds for the Central Universities (WK2340000064).

## Author information

### Author notes

1. These authors contributed equally: Fei Kong, Pengju Zhao.

### Affiliations

1. #### CAS Key Laboratory of Microscale Magnetic Resonance and Department of Modern Physics, University of Science and Technology of China (USTC), 230026, Hefei, China

• Fei Kong
• , Pengju Zhao
• , Xiangyu Ye
• , Zhecheng Wang
• , Zhuoyang Qin
• , Pei Yu
• , Jihu Su
• , Fazhan Shi
•  & Jiangfeng Du
2. #### Hefei National Laboratory for Physical Sciences at the Microscale, USTC, 230026, Hefei, China

• Fei Kong
• , Jihu Su
• , Fazhan Shi
•  & Jiangfeng Du
3. #### Synergetic Innovation Center of Quantum Information and Quantum Physics, USTC, 230026, Hefei, China

• Fei Kong
• , Pengju Zhao
• , Xiangyu Ye
• , Zhecheng Wang
• , Zhuoyang Qin
• , Pei Yu
• , Jihu Su
• , Fazhan Shi
•  & Jiangfeng Du

### Contributions

J.D. supervised the entire project. J.D., F.K., and F.S. proposed the idea and designed the experiments. F.K. and P.Z. prepared the setup and performed the experiments. X.Y. and P.Y. prepared the diamond sample. F.K. carried out the calculations. F.K., F.S., P.Z., and J.D. wrote the manuscript. All authors analyzed the data, discussed the results, and commented on the manuscript.

### Competing interests

The authors declare no competing interests.

### Corresponding authors

Correspondence to Fazhan Shi or Jiangfeng Du.

## Electronic supplementary material

### DOI

https://doi.org/10.1038/s41467-018-03969-4