Quantum State Engineering and Precision Metrology Using State-Insensitive Light Traps

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Science  27 Jun 2008:
Vol. 320, Issue 5884, pp. 1734-1738
DOI: 10.1126/science.1148259


Precision metrology and quantum measurement often demand that matter be prepared in well-defined quantum states for both internal and external degrees of freedom. Laser-cooled neutral atoms localized in a deeply confining optical potential satisfy this requirement. With an appropriate choice of wavelength and polarization for the optical trap, two electronic states of an atom can experience the same trapping potential, permitting coherent control of electronic transitions independent of the atomic center-of-mass motion. Here, we review a number of recent experiments that use this approach to investigate precision quantum metrology for optical atomic clocks and coherent control of optical interactions of single atoms and photons within the context of cavity quantum electrodynamics. We also provide a brief survey of promising prospects for future work.

Precision measurement and quantum information science (QIS) require coherent manipulations of electronic states for atoms and molecules with long decoherence times. However, photon recoils create an inevitable back-action on the atomic center-of-mass motion, hence limiting precision and control. In a deeply bound trap, atomic localization within a fraction of an optical wavelength (the Lamb-Dicke regime) greatly reduces motional effects. This capability is exemplified in the Lorentz force-based trapped ion systems with minimal perturbations to internal electronic states. The separation of internal and external dynamics is critical for precision measurement, frequency metrology, and coherent manipulations of quantum systems (1).

For neutral atoms, external trapping potentials are created from spatially inhomogeneous energy shifts of the electronic states produced by an applied magnetic, electric, or optical field. In general, such energy shifts are electronic-state dependent, and hence, atomic motion leads to dephasing of the two states. A carefully designed optical trap that shifts the energies of the selected states equally provides a solution to this problem.

Light traps employ ac Stark shifts Math introduced by a spatially inhomogeneous light field Math, where λ is the wavelength and ϵ the polarization. Two atomic states generally have different polarizabilities αi (i = 1, 2), resulting in different trapping potentials. A state-insensitive optical trap works at a specific wavelength λL and polarization ϵL, where α1L, ϵL) = α2L, ϵL) and Math (Fig. 1A). Consequently, the transition frequency ω0 between the two light-shift-modified electronic states is nearly decoupled from the inhomogeneous Math, so long as higher order contributions O(|EL|n≥4) are negligible; that is, Math, where ħ is Planck's constant h divided by 2π.

Fig. 1.

(A) Atoms inside an optical field experience energy level shifts from the ac Stark effect. When the light field is spatially inhomogeneous (a focused beam with Rayleigh range z0 and diameter w0), a light trap is formed. When the polarizabilities of states |1> and |2> are matched by appropriate choices of the light wavelength and polarization, the optical trap becomes state-insensitive. (B) Level diagram for Sr atoms. The polarizability of the ground state is determined mainly from the strong 1S0 to 1P1 resonance. The metastable triplet states are coupled to the 3S, 3D, and 5p2 3P states, with the dominant interactions given by the specific levels shown. (C) Wavelength dependence of the 1S0 and 3P0 polarizabilities, given in atomic units (a.u.) via scaling by a factor of 1/4πϵ0a30, where a0 is the Bohr radius. (D) Wavelength-dependent ac Stark shifts for the 1S0, 3P0, 3P1 (magnetic sublevel m = 0), and 3P1 (m = ±1) states, under various light polarizations (pol) and intensity I0 ∼ 10 kW/cm2.

This scenario is possible as αi(λ,ϵ) is set by multiple off-resonant atomic transitions. For alkaline earth atoms, the double valence electrons give rise to two distinct series of singlet and triplet states, and the long-lived triplet metastable states are ideal for precision spectroscopy (2). In Sr atoms (Fig. 1B), intercombination optical transitions from the ground state 5s2 1S0 to the lowest 3P0,1,2 metastable states offer narrow linewidths for clocks. The task then is to find a trapping wavelength for Math, with negligible scattering losses. For λ >461 nm, α1S0 is always positive, leading to a trapping potential at intensity maximum. For 3P0, the resonances at 2.7 and 0.68 μm make the polarizability vary from negative to largely positive as λ decreases (Fig. 1C), guaranteeing a match of α1S0 and α3P0 at a “magic” wavelength λL (solid line curves in Fig. 1D), with its value determined from many relevant electronic states with dipole couplings to 1S0 and 3P0. The shaded curves in Fig. 1D highlight the complexity due to light polarization and the vector nature of an electronic state with angular momentum J ≠ 0 (e.g., 3P1).

Equalizing light shifts using two different-colored lasers was proposed (3), and laser cooling between states of similar polarizabilities in an optical trap was discussed (4). To minimize decoherence for quantum-state manipulations, an experimental scheme emerged for a single-wavelength, far-off-resonance dipole trap (FORT) with state insensitivity (5). A magic wavelength trap allows (i) two states with the same ac Stark shifts, (ii) atoms trapped in the Lamb-Dicke regime, and (iii) atomic center-of-mass motion independent of its internal state (6). The experimental realization (7) of this proposal (8) in strong-coupling cavity quantum electrodynamics (cQED) involving the Cs 6S1/2 to 6P3/2 optical transition led to an extended atomic trap lifetime and the demonstration of diverse phenomena for the interaction of single atoms and photons (9). Unlike alkali atoms, intercombination transitions in Sr have linewidths substantially narrower than typical Stark shifts, which critically modify transition dynamics. Efficient cooling on the narrow 1S0 to 3P1 line (10) in a state-insensitive optical trap was demonstrated (11). An optical lattice clock was proposed using the ultranarrow 1S0 To 3P0 Optical Transition In 87Sr (12). The use of scalar electronic states (J = 0) allows for precise control of the Stark shifts solely by the light wavelength, a much better controlled quantity than light intensity or polarization. This is a clear advantage of a state-insensitive trap.

Thus, with independent control of atomic transition and center-of-mass motion, neutral atoms confined in state-insensitive optical traps emulate many parallel traps of single ions, creating greatly enhanced measurement capabilities and new tools for scientific investigations with quantum arrays of atoms and molecules. Two categories of work are progressing rapidly with exciting prospects: (i) precision spectroscopy and frequency metrology (1320) and (ii) quantum-state engineering in the context of cQED (9).

Precision Frequency Metrology

Lasers with state-of-the-art frequency control now maintain phase coherence for 1 s (21), and the recent development of optical frequency combs has allowed this optical phase coherence to be faithfully transferred to other parts of optical or microwave domains (5). A new generation of atomic clocks based on optical frequencies, surpassing the performance of the primary Cs standard, has been developed (20, 22). A key ingredient is the preservation of the coherence of light/matter interactions enabled by a clean separation between the internal and external degrees of freedom for trapped atoms. For Sr, the presence of a strong spin-singlet (1S0 to 1P1) transition and a weak spin-forbidden (1S0 to 3P1) transition (Figs. 1B and 3A) allows efficient laser cooling in two consecutive stages, reaching high atomic densities and low temperatures limited by photon recoils (<1 μK) (10, 23). Transitions between pure scalar states are strictly forbidden. In 87Sr, nuclear spin I = 9/2 and the resulting hyperfine interaction weakly allows the spin- and dipole-forbidden 1S0 (F = I) → 3P0 (F = I) transition (F total angular momentum) with a natural linewidth of ∼1 mHz, permitting a high quality factor for the optical resonance (16).

Precision atomic spectroscopy inside a magic-wavelength trap. With the laser-cooled atoms loaded into a one-dimensional (1D) optical standing wave (optical lattice) oriented vertically (Fig. 2), atomic spectroscopy of the 1S0 to 3P0 superposition probes the light-matter coherence at ∼1 s. The probe is aligned precisely parallel to the lattice axis to avoid transverse excitations. The Doppler effect is quantized by the periodic atomic motion and is removed by means of resolved-sideband spectroscopy where the trap frequency far exceeds the narrow transition linewidth. When the probe laser is frequency-scanned, a carrier transition appears without a change of the motional state. Blue and red sidebands result from corresponding changes of the motional states by ±1 (Fig. 2). The absence of photon recoil and Doppler effects from the carrier transition sets the stage for high-precision spectroscopy inside the lattice.

Fig. 2.

87Sr lattice clock. Blue laser light (1S0 to 1P1) is used to cool and trap Sr atoms at the center of the vacuum chamber. Atoms are further cooled with red light (1S0 to 3P1) in the second stage. Atoms are then loaded into a state-insensitive, vertical 1D optical lattice made of near-infrared light. (Top Right) Schematic levels for lattice spectroscopy, where the two electronic states are convolved with the quantized motional states. (Bottom Right) Line shape of a saturated 1S0 to 3P0 electronic transition and the motional sidebands.

Zooming into the carrier transition, 10 closely spaced resonances are observed with π excitation (Fig. 3B) under a small bias magnetic field, due to the slightly different Landé g-factors between 1S0 and 3P0. This differential g-factor, and consequently the hyperfine interaction-induced state mixing in 3P0 and its lifetime, is directly determined from the frequency gap of the resolved transitions (24). This high-resolution optical spectroscopy measures precisely the nuclear spin effects without using large magnetic fields for traditional nuclear magnetic resonance experiments.

Fig. 3.

(A) Simplified level diagram for 87Sr lattice clock. Both cooling transitions are shown, along with the clock transition. (B) Clock transition under a bias magnetic field. Linear π transitions with and without spin polarization are displayed in blue and green, respectively. (Inset) Individual nuclear spin states. After spin polarization, the population resides in a single spin state. (C) High-resolution spectroscopy of the clock π transition for a single mF state (where mF indicates magnetic sublevel), showing the ultranarrow (quality factor Q ∼ 2.4 × 1014) spectrum achieved with a 500-ms Rabi pulse. (D) Recent absolute frequency measurements of the 87Sr clock transition, with respect to Cs standards, in laboratories of JILA (blue circles), Paris (green triangles), and Tokyo (red squares). Error bars indicate ±1 SD in systematic uncertainties. The frequency is reported relative to an offset frequency ν0 = 429,228,004,229,800 Hz.

Spin polarization is implemented to consolidate the atomic population to mF = ±9/2 sublevel. For one particular mF, resonance profiles as narrow as 1.8 Hz (Fig. 3C) are observed, indicating coherent atom/light interactions approaching 1 s. The corresponding resonance quality factor is 2.4 × 1014, the highest fractional resolution achieved for a coherent system (16). The achieved spectral resolution is limited by the probe laser, with a linewidth below 0.3 Hz at a few seconds and ∼2 Hz on 1-min time scales (21).

Optical atomic clocks. The concept of a well-engineered trapping potential for accurate cancellation of the differential perturbation to the clock states has led to rapid progress in optical lattice clocks (1315), now demonstrating the high resonance quality factor, high stability (16, 18), and low systematic uncertainty (20). The high spectral resolution and high signal-to-noise ratio is a powerful combination for precision metrology. Understanding systematic uncertainties of the 87Sr lattice clock sets the stage for the absolute frequency evaluation by the primary Cs standard via an optical frequency comb. At JILA, this measurement is facilitated by a phase-stabilized fiber link that transfers atomic clock signals between JILA and NIST (25), where a Cs fountain clock and hydrogen masers are operating (26). Data accumulated over a 24-hour run allow the determination of the 87Sr 1S0 to 3P0 transition frequency at an uncertainty of 1 × 10–15, set by the statistical noise in the frequency comparison (18). In Tokyo, the frequency link to Cs reference at the National Metrology Institute of Japan uses a common view Global Positioning System carrier phase technique (17). Figure 3D summarizes (27) Sr frequency measurements relative to Cs standards in laboratories of Boulder (14, 18), Paris (15, 19), and Tokyo (17). The magic wavelength for the 87Sr 1S0 to 3P0 transition has been determined independently to be 813.4280(5) nm (17, 18, 28) and, as expected (12), sharing its value at 7 significant digits is sufficient to provide a 15-digit agreement of the clock frequency among the three continents, demonstrating the reproducibility of optical lattice clocks and the success of a new kind of atomic clocks with engineered perturbation.

Under the current operating conditions, the Sr lattice clock has a quantum-projection–noise-limited instability <1 × 10–15 at 1 s, which is somewhat degraded by insufficient stability of the optical local oscillator. With this high measurement precision, rigorous evaluations of the overall uncertainty of an optical atomic clock now demand direct comparison against other stable optical clocks. Stable optical frequencies can be transferred over many kilometers by means of a phase-stabilized fiber link with a stability of 1 × 10–17/√τ (where τ is averaging time) (25), permitting evaluation of systematic uncertainties of the JILA Sr clock by remote comparisons against a Ca optical clock at NIST. The overall systematic uncertainty of the Sr lattice clock is currently evaluated near 1×10–16 (20). The low measurement uncertainty achieved in large ensembles of atoms is a powerful testimony to the importance of state-insensitive traps.


An important advance in modern optical physics has been the attainment of strong coupling for the interaction of single atoms and photons. The principal setting for this research has been cQED, in which an atom interacts with the electromagnetic field of a high-Q resonator to investigate fundamental radiative processes associated with the strong interaction of one atom and the electromagnetic field (5), with applications in quantum optics and QIS (29).

Various approaches to trap and localize atoms within high-finesse optical cavities have been developed over the past decade, with the goal of achieving well-defined coupling g0 between atom and cavity field, where 2g0 is the Rabi frequency for a single photon. Beyond atomic confinement per se, it is also important that the mechanism for trapping should not interfere with the desired cQED interactions for the relevant atomic transitions (for instance, |b〉 ↔ |e〉 in Fig. 4A) [see section 3 in (5)].

Fig. 4.

(A) Illustration of the protocol of (30) for the distribution of quantum states from system A to system B by way of atom/photon interactions in cQED. As shown in inset (i), at system A, the external control field Ω1(t) initiates the coherent mapping of the atomic state |ψ〉 = ca|a〉 + cb|b〉 to the intracavity field by way of the coupling g and thence to a propagating pulse via the cavity output mirror with coupling κ. |a〉 and |b〉 indicate two long-lived atomic ground states. At the second cavity B, the control field Ω2(t) implements the reverse transformation as in inset (ii), with the incoming pulse from A coherently transformed back to |ψ〉 for the atom at B. By expanding to a larger set of cavities connected by fiber optics, complex quantum networks can be realized. (B) Level diagram for the atom-cavity system showing the lowest energy manifolds with n = 0,1,2 for an atom of transition frequency ωA coupled to a cavity with resonance frequency ωC, with ωA = ωC ≡ ω0. Displayed is the eigenvalue structure for the (6S1/2, F = 4, mF) ↔ (6P3/2, F′ = 5, mF′) transition in Cs [corresponding to |b〉 ↔ |e〉 in (A)] for coupling with rate g0 to two degenerate cavity modes with orthogonal polarizations. The basis for photon blockade for an incident probe field of frequency ωp is the suppression of two-photon absorption for the particular detuning ωp shown by the arrows. Single photons are transmitted for the transition from the ground to the lowest excited manifold (i.e., n = 0 to n = 1), but photon pairs are “blocked” because of the off-resonant character of the second step up the ladder (i.e., n = 1 to n = 2) (38). (C) Experimental arrangement for trapping one atom with an intracavity FORT operated at the magic wavelength λL = 936 nm for one mode of the cavity and driven by ϵFORT (32). Cooling of the radial atomic motion is accomplished with the transverse fields Ω4, whereas axial cooling results from Raman transitions driven by the fields ϵFORT, ϵRaman. The cavity length l = 42 μm, and the waist w0 = 24 μm. cQED interactions take place near a second cavity mode at λ0 = 852 nm. (D) Transmission spectrum T1p) and intracavity photon number 〈np)〉 versus frequency ωp of the probe beam ϵp for an individual strongly coupled atom, as in (C) (35). T1p) is acquired for one-and-the-same atom, with the two peaks of the vacuum-Rabi spectrum at ωp/2π = –20, +32 MHz in correspondence to the splitting for the lower (n = 1) manifold of states in (B). The asymmetry of the spectrum arises from tensor shifts of the mF excited states in the FORT. The small auxiliary peaks are from the distribution of Clebsch-Gordon coefficients for the (6S1/2, F = 4, mF) ↔ (6P3/2, F′ = 5, mF′) transitions. The full curve is from the steady-state solution to the master equation (35). Error bars represent ±1 SD from the finite number of recorded photo-counts.

The trapping scheme should also support confinement and long coherence times for auxiliary atomic states (e.g., |a〉↔|b〉 in Fig. 4A). For example, the initial proposal for the implementation of quantum networks (30) achieves a quantum interface between light and matter via cQED. “Stationary” qubits are stored in the states |a〉 and |b〉 and are locally manipulated at the nodes of the network. Coherent coupling g to the cavity field and thence to “flying” qubits between system A and system B is provided for one leg of the transition (|e〉 ↔ |b〉), with an external control field Ω(t) exciting the second leg (|e〉 ↔ |a〉) in a “STIRAP” (Stimulated Raman Adiabatic Passage) configuration. Often, |a〉 and |b〉 are hyperfine states (e.g., the “clock” transition F = 3, mF = 0 ↔ F = 4, mF = 0 in the 6S1/2 level in Cs), whereas |e〉 is an excited electronic state (for instance, in the 6P3/2 manifold in Cs).

cQED and the magic wavelength. In contrast to precision metrology, where the goal is to isolate a particular atomic transition from external perturbations, strong coupling in cQED explicitly introduces large perturbations to the relevant atomic and cavity states. Indeed, for n quanta, the composite eigenstates for a two-state atom coupled to the cavity field experience frequency shifts Math, as illustrated in Fig. 4B for the n = 1,2 manifolds. Moreover, in addition to strong coupling for the internal degrees of freedom of the atomic dipole and cavity field [i.e., Math, with (γ, κ) the decay rates for atom and cavity], single quanta can also profoundly influence the external, center-of-mass degree of freedom, Math, with Ek the atomic kinetic energy. Finally, it is possible to interrogate the atom-cavity system at rates exceeding γ ∼108 s–1 for an allowed dipole transition, with potentially large heating. This situation differs markedly from the more leisurely inquires employed for frequency metrology with a forbidden transition, for which γ ∼1 s–1.

In general, the atom-cavity coupling Math and the ac-Stark shifts Math and Math for excited and ground states (e, g) have quite different form and magnitude, resulting in a complex spatial structure for the transition frequencies of the atom-cavity system, as discussed in more detail in section 2 in (5). In contrast, in a FORT at λL, Math, so that the dressed states of the atom-cavity system revert to their basic form Math with dependence only on Math. From a pragmatic perspective, a great benefit of a FORT operating at λL is that the powerful techniques for laser cooling and trapping of neutral atoms in free space can be taken over en masse to the setting of cQED.

Strong coupling for one atom in a state-insensitive trap. The initial realization of trapping of a single atom inside a high-Q cavity in a regime of strong coupling employed a conventional FORT (i.e., Math) with a trap lifetime τ ≈ 30 ms (6). State-insensitive trapping was achieved later for single Cs atoms stored in a FORT operated at the magic wavelength λL = 935.6 nm (7). The observed lifetime of τ ≈ 3 s represented an advance of 102 to 104 for trapping in cQED (6, 31). Moreover, Sisyphus cooling (32) for a strongly coupled atom was made possible by Math. Independent investigations of trapping Cs in free-space FORT around the magic wavelength were reported (33).

The combination of strong coupling and trapping at the magic wavelength enabled rapid advances in cQED (9). Included are the realization of a one-atom laser in the regime of strong coupling, the efficient generation of single photons “on demand,” the continuous observation of strongly coupled and trapped atoms (7, 34), and the observation of the vacuum-Rabi splitting ±g0 (35). The experiment in (35) (Fig. 4C) is important in that technical capabilities built around a magic wavelength FORT allowed for a rudimentary quantum protocol with “one-and-the-same” atom, as shown in Fig. 4D. In contrast, all earlier experiments related to strong coupling in cQED had required averaging over ∼103 to 105 single-atom trials. Essential components of this work were the state-insensitive FORT and a new Raman scheme for cooling to the ground state of axial motion (36). The implementation of complex algorithms in QIS requires this capability for repeated manipulation and measurement of an individual quantum system [e.g., for the generation of single photons (37)].

The experimental arrangement depicted in Fig. 4C has also enabled strong photon/photon interactions, as manifest in the phenomenon of photon blockade (38). The underlying mechanism is the anharmonicity of the energy spectrum for the atom-cavity system illustrated in Fig. 4B, which arises only for strong coupling and closely mirrors the free-space structure in a FORT at the magic wavelength. Reversible mapping of a coherent state of light to and from the hyperfine states |a〉 and |b〉 of an atom trapped within the mode of a high-finesse optical cavity (Fig. 4A) has also been achieved (39), thereby demonstrating a fundamental primitive for the realization of cQED-based quantum networks (29, 30).

Atomic localization in cQED. Trapping single atoms within high-Q cavities has led to diverse advances in optical physics, including new regimes for optical forces not found in free space (4044). Initially, the principal mechanism for trapping was a red-detuned FORT operated relatively close to atomic resonance, for which Math where Math is the trapping potential for the atomic ground state b in Fig. 4A] with correspondingly limited trapping times ≤0.1 s (6, 4345). More recently, λF (the FORT wavelength) has been shifted beyond 1 μm, and much longer trap lifetimes ∼10 s have been achieved (37, 46), as well as the deterministic transport of single atoms into and out of the cavity (47).

Strong coupling with trapped ions is an exciting prospect as the trapping potential for the atomic motion is independent of internal states and trapping times are “indefinite.” Although great strides have been made (48, 49) and the boundary for strong coupling reached (49), an inherent conflict is between small mode volume and stable trapping.

Future Prospects

Precision quantum metrology. Alkaline earth atoms confined in state-insensitive lattice traps provide a fertile playground for quantum optics and precision measurement–based quantum metrology. Although challenging, the precision of atomic spectroscopy will probably reach the limit set by quantum projection noise. This is an important milestone for large ensembles of atoms and will enable atomic clocks to operate with unprecedented stability. With continued improvement of stable lasers, tomorrow's optical lattice clocks will exhibit instabilities below 10–16 at 1 s. Quantum nondemolition measurement for spin-squeezing in an optical lattice can prepare a collective macroscopic pseudo-spin to further enhance the clock stability and precision. High measurement precision will be critical for the evaluation of systematic uncertainties of these new clocks. For example, systematic uncertainties <1 × 10–17 would require evaluation times of only a few hundred seconds.

The idea of state-insensitive traps extends to zero nuclear-spin bosonic isotopes of Sr, Yb, or others by using external fields to induce forbidden transitions (50, 51). Application of group IIb elements (Zn, Cd, and Hg) for optical lattice clocks will significantly reduce the sensitivity to the blackbody radiation–induced shift. Recently, magneto-optical trapping of Hg was reported (52). State-insensitive optical traps also benefit research on cold molecules, with important directions toward novel quantum dynamics, precision measurement, and ultracold chemistry. The scalar nature of molecular vibrational levels in the electronic ground state simplifies the search for a magic wavelength for matching polarizabilities between two specific vibrational levels, creating a high-accuracy optical molecular clock (53). This molecular system is attractive for searching possible time variations of fundamental constants, particularly the electron/proton mass ratio. Comparison among these different clocks will diversify and strengthen tests of the laws of nature.

The combination of quantum manipulation and precision metrology in an optical lattice allows for accurate assessment of the system's quantum coherence while maintaining precise control of interparticle interactions. Quantum statistics of nuclear spins can be used to turn electronic interactions on and off. Meanwhile, couplings between nuclear spins in the lattice can be enhanced via electronic dipolar interactions. These electronic interactions are accessed through narrow-linewidth optical Feshbach resonances (54) and may allow entangling nuclear spins. These tunable interactions are ideal for QIS, where qubits are strongly coupled to one another on demand but weakly coupled to the error-inducing environment. Furthermore, individual nuclear spins may be addressed and monitored with the use of high–spectral resolution optical probes under an inhomogeneous magnetic field. Non-uniform properties of an optical lattice can thus be probed and compensated with spatial addressing.

Applications of state-insensitive traps in QIS. Recently, quantum degenerate atomic gases have been trapped and strongly coupled to optical cavities (5557), with a variety of atomic collective effects explored. Another area of considerable activity has been the interaction of light with atomic ensembles (that is, a large collection of identical atoms), with important achievements reported for both continuous quantum variables and discrete excitations (58). In these areas and others, state-insensitive optical traps can enable new scientific capabilities by minimizing the role of decoherence while at the same time allowing coherent optical interactions mediated by electronic excited states. Of particular interest are the implementation of quantum networks and the exploration of the quantum limits to measurement.

Quantum networks. Quantum state transfer (Fig. 4A) provides a basis for implementing complex quantum networks (30). However, experiments in cQED have relied on Fabry-Perot cavities formed by two spherical mirrors. There have been intense efforts to develop alternative microcavity systems (5962) for scalable quantum networks and quantum information processing on atom chips (61). A candidate for trapping individual atoms near a monolithic microcavity is a FORT operated at two magic wavelengths—one red and the other blue, detuned from resonance (63).

With respect to atomic ensembles (58), there is clearly a need to extend coherence times for stored entanglement, where currently τ ∼10–5 s for entanglement of single excitations between remotely located ensembles. A promising mechanism is confinement of atoms within a state-insensitive trap to realize a long-lived material system for the nodes of a quantum network (64). In this setting, dephasing because of position-dependent shifts in transition frequency within the trap is minimized.

Quantum measurement. We have previously discussed the prospects for surpassing the limit set by quantum projection noise for precision spectroscopy. In addition to this important possibility, there are other applications of state-insensitive traps to quantum measurement, particularly within the setting of cQED. For example, by separating the functions of trapping (via a state-insensitive FORT) and sensing (by way of a probe field in cQED), it should be possible to confront the quantum limits for real-time detection of atomic motion, including localization beyond the standard quantum limit. The broader context of such research is that of the dynamics of continuously monitored quantum systems, whereby the strong coupling of atom and cavity implies a back reaction of one subsystem on the other as a result of a measurement (65).

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