Complete polarization control for a nanofiber waveguide using directional coupling

TL;DR

This paper introduces a novel nanofiber directional coupler that enables complete polarization control with high fidelity, overcoming the inherent polarization maintenance limitations of optical nanofibers.

Contribution

The work presents a new crossed nanofiber coupler design that allows for precise polarization state preparation and control along a nanofiber waveguide.

Findings

Achieved polarization state preparation with >99% fidelity.

Demonstrated complete polarization control method.

Validated directional coupling based on asymmetric dipolar emission.

Abstract

Optical nanofiber waveguides are widely used for near-field delivery and measurement of light. Despite their versatility and efficiency, nanofibers have a critical drawback - their inability to maintain light's polarization state on propagation. Here, we design a directional coupler consisting of two crossed nanofibers to probe the polarization state at the waist region. Directionality of coupling occurs due to asymmetric dipolar emission or spin-locking when the evanescent field pattern breaks the mirror symmetry of the crossed-nanofiber system. We demonstrate that, by monitoring the outputs from the directional coupler, two non-orthogonal polarization states can be prepared at the nanofiber waist with a fidelity higher than 99%. Based on these states, we devise a simple and reliable method for complete control of the polarization along a nanofiber waveguide.

Equations

$$\mathbf{E}(z)=\alpha (z){\mathbf{HE}}_{11}^x+\beta (z){\mathbf{HE}}_{11}^y,$$

$$\mathbf{j}=\frac{1}{\sqrt{|\alpha {|}^2+|\beta {|}^2}}\left[\begin{array}{c}\alpha \\ \beta \end{array}\right].$$

$$\mathbf{j}(z)=u_{\mathrm{fiber}}\mathbf{j}(z_0),$$

$$u_{\mathrm{fibre}}^{†}{u}_{\mathrm{fibre}}=\mathrm{I},$$

$$P_{\Sigma }=(P_{+}+P_{-})\propto (\cos 2\psi +\mathrm{const}),$$

$$P_{\Delta }=(P_{+}-P_{-})\propto \sin 2\chi ,$$

$$\{\begin{array}{l}u\mathbf{A}={\mathrm{e}}^{i{\delta }_A}\mathbf{A}\\ u\mathbf{B}={\mathrm{e}}^{i{\delta }_B}\mathbf{B}\end{array},$$

$$⟨\mathbf{A}|u^{†}u|\mathbf{B}⟩=⟨\mathbf{A}||\mathbf{B}⟩={\mathrm{e}}^{i({\delta }_A-{\delta }_B)}⟨\mathbf{A}||\mathbf{B}⟩.$$

$$⟨\mathbf{A}|\mathbf{B}⟩\ne 0,$$

$$\{\begin{array}{l}\mathbf{C}=a\mathbf{A}+b\mathbf{B}\\ u\mathbf{C}={\mathrm{e}}^{i\delta }\mathbf{C}\end{array},$$

Full text

I I. Introduction

Tapered optical fibers are unique because they allow for the smooth transition of light from macro- to micro- or nanoscale systems. Owing to the strong evanescent field around the ultrathin waist region, such fibers are efficient and versatile tools for optical manipulation Brambilla et al. (2007); Maimaiti et al. (2015); Ren et al. (2016), sensing Yoshie et al. (2011); Yu et al. (2014), nonlinear optics Beugnot et al. (2014); Zoubi and K. Hammerer (2017), microcavities Cai et al. (2000), atomic physics Le Kien et al. (2004); Hendrickson et al. (2010); Vetsch et al. (2012); Kumar et al. (2015); Kornovan et al. (2017), and various studies of light-matter interactions in both classical and quantum regimes Guo et al. (2009); Tong et al. (2012); Solano et al. (2017). As light propagates from the fiber pigtail to the waist region (Fig. 1(a)), the mode volume reduces, and the intensity of the evanescent field increases Le Kien et al. (2004). Optical power can be transferred to the waist without significant losses, even for ultrathin fibers. However, the other important parameter of the field—its polarization—is usually impossible to control. The polarization of the evanescent field is crucial for many nanofiber-based studies including microcavity mode excitation Knight et al. (1997) and interactions with nanoparticles Wang et al. (2007) or atomic ensembles Nieddu et al. (2016); Sadgrove et al. (2016).

As simple as it may seem, the problem of polarization uncertainty in tapered fibers has challenged the scientific community for decades. To solve it, one must establish a direct link between the near field at the ultrathin waist and the far field where macroscopic detectors and controllers are typically placed. In this work, we explore directional coupling between two crossed nanofibers, and, consequently, develop a reliable method for achieving an arbitrary polarization state in the evanescent field of a single-mode nanofiber. The physics behind this directionality features the interplay of two phenomena: the well-known spin-momentum locking, and the newly found mirror-symmetry breaking of a light-matter system by an induced electric dipole.

We begin by introducing optical nanofibers and their fabrication in Sec. II, and discuss how the polarization of light propagates in adiabatically tapered fibers. We emphasize that the polarization transformation in such fibers, as in any optical elements free of depolarization and dichroism, is equivalent to rotations of the Poincaré sphere. In Sec. III, we devise a simple, two-step procedure, which allows for reversing the above rotational transformations via consecutive mapping of two non-orthogonal polarization states. By compensating an arbitrary transformation, one achieves complete control over the polarization state. Section IV is dedicated to the directional coupling between two single-mode optical nanofibers crossed at right angles. We present a detailed experimental and numerical study of the directional coupler’s operation. The results indicate how to securely identify a pair of non-orthogonal states required for the two-step compensation procedure to be applicable in the case of a nanofiber waveguide. Section V presents a practical demonstration of the polarization control. We discuss its precision and accuracy, as well as the experimental evidence related to polarization evolution in a tapered optical fiber.

II II. Polarization of light in a nanofiber waveguide

Nanofibers are generally produced from conventional optical fibers by controlled heating and pulling (Ward et al., 2014). A typical, single-mode nanofiber consists of a cylindrical submicron-diameter waist connected to fiber pigtails by two taper regions, see Fig. 1(a), where the Cartesian coordinate system $(x,y,z)$ originates in the middle of the waist and $z$ is parallel to the fiber axis. For this work, the tapered fibers were prepared from a step-index cylindrical optical fiber with a cut-off wavelength of $920\pm 50$ nm. The cylindrical waist regions were about 2 mm long with radii of $159\pm 3$ nm, as measured by a scanning electron microscope. The input pigtail was coupled to a collimated Gaussian beam from a continuous wave laser (980 nm wavelength). Each fiber was kept as short, straight, and strain-free as possible. Such precautions are common practice in nanofiber experiments where polarization (or mode) transformations are undesirable.

The key questions to be addressed are (i) how does the polarization of guided light change upon propagation through a tapered fiber? and—more importantly—(ii) how can this change be controlled? A polarization state can be treated as a unit vector ${\bf s}=(1,S_{1},S_{2},S_{3})$, where $S_{1,2,3}$ are the Stokes parameters which define a point on the Poincaré sphere, $\cal P$, see Fig. 1(b). The azimuthal ($2\psi$) and polar ($2\chi$) angles on the sphere are directly linked to the orientation, ellipticity, and handedness (through the sign of $\chi$) of the polarization ellipse traced in the $(x,y)$ plane by the tip of the electric field vector, ${\bf E}(t)$, see Fig. 1(c), in the following way: ${\bf s}=(1,\cos 2\psi\cos 2\chi,\sin 2\psi\cos 2\chi,\sin 2\chi)$.

First, we compared the polarization state at the input, ${\bf s}_{\rm in}$, and the output, ${\bf s}_{\rm out}$, of our tapered fibers. In order to probe a large part of $\cal P$, ${\bf s}_{\rm in}$ was driven around the Poincaré sphere in a figure-of-eight trajectory by passing the horizontally-polarized ($\bf H$) input beam through a rotating quarter-wave plate (QWP). The trajectory was recorded by means of a commercial polarization analyzer. For every fiber under test, the output trajectory repeated the shape of the input, but always exhibited a significant shift on the sphere (see a typical example in Fig. 1(b)), regardless of our efforts to maintain the polarization using the fore-mentioned precautions.

To understand how the shape of the trajectory on $\cal P$ is maintained, let us note that the fibers were designed according to the adiabatic condition which implies energy transfer with minimum loss. Adiabaticity was ensured by keeping the taper angle below the critical value Love et al. (1991); Jung et al. (2008) and the transmission at 980 nm wavelength above 97% throughout the pulling process. Both pigtails and the cylindrical waist region are single-mode, hence losses can only occur in the tapers via coupling to radiation modes and higher-order modes which cannot propagate along the single-mode fiber. The guided electric field, ${\bf E}(z)$, in adiabatic single-mode fibers can be described as a combination of two orthogonal, quasi-linearly polarized fundamental eigenmodes, ${\bf HE}_{11}^{x}$ and ${\bf HE}_{11}^{y}$ Le Kien et al. (2004):

[TABLE]

where $\alpha$ and $\beta$ are variable complex amplitudes. The polarization ellipse is associated with the Jones vector

[TABLE]

Its evolution upon propagation from $z_{0}$ to $z$ through the fiber can be written as

[TABLE]

and, given that adiabatic fibres have transmission close to unity, $u_{\rm fibre}$ must be a $2\times 2$ unitary matrix:

[TABLE]

where $\rm I$ is the identity matrix. Therefore, transformations of the Stokes vectors in adiabatically-tapered fibers are restricted to the 3D rotation (SO(3)) group Sakurai (1994). Rotations of the Poincaré sphere (${\cal P}\to{\cal P}^{\prime}$) preserve angles between the Stokes vectors, and, consequently, the shape of the trajectories for ${\bf s}_{\rm in}$ and ${\bf s}_{\rm out}$ in Fig. 1(b). This preservation of angles is the key condition for the polarization control that we achieve.

III III. Two-step polarization compensation

The polarization state at the nanofiber waist, ${\bf s}_{\rm w}$, can be linked to the input and output states in terms of Mueller calculus Chipman (2010): ${\bf s}_{\rm w}={\rm M}_{-}{\bf s}_{\rm in}$, and ${\bf s}_{\rm out}={\rm M}_{+}{\bf s}_{\rm w}$, where ${\rm M}_{-}$ and ${\rm M}_{+}$ are $4\times 4$ matrices describing the Stokes vector evolution before ($z<0$) and after ($z>0$) the waist. These two matrices do not correlate and cannot be determined if one only measures ${\bf s}_{\rm in}$ and ${\bf s}_{\rm out}$. Consequently, in order to control ${\bf s}_{\rm w}$, one has to probe the evanescent field.

Theoretically, ${\rm M}_{-}$ can be found by measuring several sets of (${\bf s}_{\rm in}$, ${\bf s}_{\rm w}$) Chipman (2010). However, this procedure is not always realistic. Instead of controlling the target polarization state by deducing ${\rm M}_{-}$, in this work we followed a different strategy, which is more practical and, as will become clear, is the only option for nanofiber waveguides. Namely, we reverse the transformation of the Poincaré sphere, ${\cal P}\to{\cal P}^{\prime}$, thus achieving ${\cal P}\to{\cal P}$ and ${\bf s}_{\rm w}={\bf s}_{\rm in}$.

From a geometrical point of view, the orientation of a sphere can be completely defined by two independent angles, i. e., latitude and longitude. It is, therefore, logical to realize the ${\cal P}\to{\cal P}$ mapping in two steps:

tilting of one axis by an angle $\varphi_{1}$ (Fig. 2(a)); 2. 2.

rolling of the two other axes about the first one by an angle $\varphi_{2}$ (Fig. 2(b)).

Importantly, this two-step procedure for reversing unknown polarization transformations is not restricted to nanofibers, but can be applied to any optical element free of depolarization and dichroism. In practice, we realized the procedure by means of a free-space polarization compensator (PC) consisting of a variable retarder (VR, with the fast axis parallel to $x$) and a pair of quarter-wave plates (${\rm WP}_{1,2}$), see Fig. 2(c). The compensator is characterized by an unitary Jones matrix, $u_{\rm PC}$, or a Mueller matrix, ${\rm M}_{\rm PC}$. In step (1), ${\rm WP}_{1}$ and ${\rm WP}_{2}$ are independently rotated until the input horizontal polarization (${\bf s}_{\rm in}={\bf H}$; $S_{1}=1$) is mapped onto itself at the nanofiber waist (${\bf s}_{\rm w}={\bf H}$; $S_{1}^{\prime}=1$). Next, in step (2), an input state with $|S_{1}|\neq 1$ is selected, and the retardance of VR is adjusted. This drives ${\bf s}_{\rm w}$ along the circle in the plane parallel to $(S_{2},S_{3})$ until eventually $S_{2,3}^{\prime}=S_{2,3}$, and thus ${\bf s}_{\rm w}={\bf s}_{\rm in}$ due to ${\rm M}_{\rm PC}={\rm M}_{-}^{-1}$. In fact, ${\cal P}\to{\cal P}$ mapping can be performed with any pair of non-orthogonal states, i. e. such states that do not lie on the same diameter of the Poincaré sphere, or—in mathematical terms—have a non-zero inner product (see the proof in Appendix).

IV IV. Crossed-nanofiber directional coupler

In practice, to identify two non-orthogonal polarization states at the waist of a nanofiber, we cross it with a near-identical nanofiber at right angles, as sketched in Fig. 3(a). Near-field probing one (input) ultrathin fiber with another (output) one is not new, see for instance its application for the purpose of profilometry Madsen et al. (2016); Fatemi et al. (2017). In this work, for the first time, we consider symmetry of such a system (hence the importance of the right-angle crossing) and use output signals from both ends of the probe fiber. The efficiency of near-field coupling to guided modes which produce these signals is very low, typically under $0.1\%$, see Fig. 6(d),(e). However, it is sufficient for unambiguous identification of non-orthogonal $\bf H$ and ${\bf R}_{\rm M}$ (see below) polarization states at the waist of the input fiber.

The system of two crossed fibers has a symmetry plane, $(x,z)$, shown as the dash-dotted line in Figs. 3(b),(c). When the input beam is $\bf H$- or $\bf V$-polarized, the overall symmetry of the light-matter system is preserved and the optical power values, $P_{+}$ and $P_{-}$, measured at the ends of the output fiber, are equal: $P_{+}=P_{-}$. Otherwise, the symmetry is broken and in general $P_{+}\neq P_{-}$. Interestingly, this directional coupling of light can be separated into two independent effects associated with orientation ($\psi$) and shape ($\chi$) of the polarization ellipse. Let us now consider the two special cases of linear ($\psi\neq{\rm const}$; $\chi=0$) and circular ($\chi=\pm\pi/4$) polarizations.

For a tilted linear polarization (Fig. 3(b)), the mirror symmetry is broken by the emission pattern of an electric dipole induced at the crossing point. As a result, two counter-propagating modes of non-equal power are generated in the output fiber. A wave with reflection angle, $\theta$, carries energy proportional to $\sin^{2}(\theta+\psi)$. Assuming that all angles allowed in this nanofiber equally contribute to the energy transfer, the net power radiated along the $\pm$ direction is proportional to $\int_{\theta_{\rm c}}^{\pi/2}\sin^{2}(\theta\pm\psi)d\theta$, where $\theta_{\rm c}$ is the critical angle. Therefore, the output power sum,

[TABLE]

which has a maximum (minimum) for ${\bf H}$ (${\bf V}$) polarization. This effect, which we dubbed “asymmetric dipolar emission” in order to emphasize its geometrical origin, provides an alternative way to achieve directionality without spin-momentum locking Picardi et al. (2018). This possibility has been overlooked in earlier works on directional coupling in similar systems Petersen et al. (2014); Sadgrove et al. (2017).

For circular polarization, the electric field vector, ${\bf E}(t)$, traces a circle about the longitudinal axis, $z$, see Fig. 3(c). In free space, such a field only contains the longitudinal component of the photon spin, ${\bf J}_{z}$. The evanescent field may also contain a significant transverse spin component, ${\bf J}_{\rm trans}$, which appears due to interaction between the real, ${\rm Re}({\bf k})$, and imaginary, ${\rm Im}({\bf k})$, parts of the wave vector, $\bf k$, at the interface between two different media Bliokh et al. (2015a). Interestingly, ${\rm Re}({\bf k})$, ${\rm Im}({\bf k})$, and ${\bf J}_{\rm trans}$ must form a right-handed system Van Mechelen and J. Zubin (2016). As a result, the direction of ${\bf J}_{\rm trans}$ defines the direction of the propagating wave Petersen et al. (2014); O’Connor et al. (2014). This phenomenon is known as “spin locking” or the “quantum spin Hall effect” of light Bliokh et al. (2015b). With regard to our crossed nanofibers, spin locking causes $P_{-}\neq P_{+}$, since the vector ${\bf J}_{z}$ is simultaneously the longitudinal spin for the input nanofiber and the transverse spin for one of the counter-propagating, $x$-polarized modes of the output nanofiber. Simple trigonometric considerations yield that the output power difference produced by the spin locking effect,

[TABLE]

with maximum and minimum values at $\chi=\pi/4$ (${\bf R}$ polarization state) and $\chi=-\pi/4$ (${\bf L}$ state), respectively.

For elliptical polarization ($\psi,\chi\neq 0$), both asymmetric dipolar emission and spin locking effects may influence the output power balance. In order to confirm the above analytical predictions for the special cases and generalize the understanding of the directional coupler’s operation, finite-element numerical simulations of $P_{\pm}$ for ${\bf s}_{\rm w}$ covering the whole Poincaré sphere were performed. The results for variable $\psi$ and $\chi$ are shown in Figs. 4(a),(b) 111For the ease of presentation, this figure shows experimental data collected after the polarization compensation.. The insets in Fig. 4(a) demonstrate that $\bf H$ and $\bf V$ correspond to the global extrema of $P_{\Sigma}$ and each of these two states can be identified and used in the first step of the polarization compensation. Experimentally, $\psi$ was varied while keeping $S_{3}=0$ by sending the $\bf H$-polarized input beam through a rotating half-wave plate (HWP). The data (diamonds) agree with the simulation (solid curve). Thus, $P_{\Sigma}$ can be readily used for ${\bf H}\to{\bf H}$ mapping, which can be further verified by monitoring the intensity of scattering from the fiber crossing, $I$, see the experimental (dots) and theoretical (dashed curve) results in Fig. 4(a). We measured $I$ as the total brightness of the camera image captured through a linear polarizer parallel to the $y$ axis Vetsch et al. (2012).

The simulations of $P_{\Delta}$ (see insets in Fig. 4(b)) reveal that, due to the interplay between the asymmetric dipolar emission and the spin locking effects, the global maximum (minimum) of $P_{\Delta}$ is shifted from the expected $\bf R$ ($\bf L$) to ${\bf R}_{\rm M}$ (${\bf L}_{\rm M}$) by $\Delta\chi\approx 8^{\circ}$. This value depends on the radii of the nanofibers and was under $10^{\circ}$ for the region where significant coupling can be achieved (see Fig. 5(b) and Figs. 6(d),(e)). Experimentally, $\chi$ was varied while keeping $S_{1}=0$ by rotation of a HWP in front of a QWP fixed at $45^{\circ}$ to the $x$ axis, as depicted in Fig. 8(g). In order to avoid systematic errors associated with $\Delta\chi$, in the second step of the polarization control, we mapped ${\bf R}_{\rm M}\to{\bf R}_{\rm M}$ instead of ${\bf R}\to{\bf R}$.

All data presented in Fig. 4 were collected while keeping the fiber crossing point fixed. Now let us check whether the choice of the crossing point makes a difference. For instance, if the polarization at the input fiber waist depends on the longitudinal position, $z$, the curves for $P_{\Sigma,\Delta}$ versus the HWP orientation, $\varphi_{\rm HWP}$, will have variable phase shifts. Alterations to $P_{\Sigma,\Delta}$ will also appear if the directional coupling depends on the vertical position of the output fiber, or, effectively, its radius at the crossing. We tested both possibilities using one period of the ${\bf HRVL}$ trajectory on the Poincaré sphere (Figs. 8(d),(f)). First, we displaced the output fiber along its axis, thus varying $\Delta y=(y-y_{0})$ while keeping the longitudinal position of the crossing point fixed, so that $\Delta z=(z-z_{0})={\rm const}$, where $y_{0}$, $z_{0}$ are random initial coordinates. As shown in Fig. 6(a), the measured $P_{\Delta}$ is independent of $\Delta y$, up to an amplitude scaling factor. The same behavior was observed when the crossing point was displaced along $z$ with $\Delta y={\rm const}$, see Fig. 6(b). These results indicate that ${\bf s}_{\rm w}$ is maintained throughout the coupling region, which we define as the $y\times z$ area where light can still couple to the output fiber. We found that the amplitudes of $P_{+}$ and $P_{-}$ are nonzero within $4$ mm$\times 4$ mm area covering the waist and thinner parts of the tapers, see the radius profile in Fig. 6(c).

According to our numerical simulations presented in Fig. 6(d), the coupling efficiency, $\eta=P_{\Sigma}/P_{\rm T}$ (where $P_{\rm T}$ is the optical power transmitted through the input fiber) is maximum for an input nanofiber radius, $r_{\rm in}^{\rm max}\approx 210$ nm, and an output nanofiber radius, $r_{\rm out}^{\rm max}\approx 220$ nm. We have measured $\eta$ over the whole coupling range with a step of 0.25 mm in $y$ and $z$. The resulting efficiency map shown in Fig. 6(e) agrees reasonably with the simulations. Notably, the whole explored range for the nanofiber radii, $r$, corresponds to the single-mode regime, since the normalized frequency parameter, $V=(2\pi r/\lambda)\sqrt{1.45^{2}-1}<2.356$, is below the cut-off value of 2.405 Snyder and J. D. Love (1983). In fact, the polarization compensation is valid only for single-mode input nanofibers, with a minimum wavelength-to-diameter ratio of $\pi$NA$/2.405$ (about 1.372 for glass in air).

V V. Polarization control

Figure 7 illustrates the precision of the polarization control we achieved. In order to estimate the precision, the input pigtail was spliced to fiber paddles (Fig. 2(c)) that allowed us to produce a random ${\rm M}_{-}$. For each random setting of the paddles, the two-step compensation procedure was performed by ${\bf H}\to{\bf H}$ and ${\bf R}_{\rm M}\to{\bf R}_{\rm M}$ mapping. Then, ${\bf s}_{\rm out}$ was measured for the three principal states: ${\bf H}$, ${\bf D}$, and ${\bf R}$. The resulting statistics over 26 sets (see Fig. 7(a)) gives the following deviations from the mean: $1.16\pm 1.43^{\circ}$, $6.03\pm 3.82^{\circ}$, and $4.29\pm 2.37^{\circ}$ for H, D, and R, respectively. The fidelities (defined as the cosine of the mean angular distances) for these states are 0.9998, 0.9945, and 0.9972, respectively. The offsets from the target states (about $10^{\circ}$ for this fiber) are due to the unknown, constant matrix ${\rm M}_{+}$.

Besides the principal states, the method was tested for a figure-of-eight trajectory (black diamonds and dotted line in Fig. 1(b) and Fig. 7(b)). The randomly arranged paddles could move the uncompensated trajectory to any part of the sphere (see the blue solid curve in Fig. 7(b) as an example). Compensation with ${\bf H}\to{\bf H}$ and ${\bf R}_{\rm M}\to{\bf R}_{\rm M}$ brings the trajectory (red filled squares) close to the initial one. This result indicates that the second (straight) part of the tapered fiber (corresponding to ${\rm M}_{+}$) contributed only a minor transformation to ${\bf s}_{\rm w}$. The case where the correction to $\Delta\chi$ is ignored was also checked. In this case, the initial state is ${\bf R}$, and ${\bf R}\to{\bf R}_{\rm M}$ mapping is achieved by locating the maximum of $P_{\Delta}$. This mapping causes systematic errors for $\varphi_{2}$, see the compensated trajectories in Fig. 7(b).

In order to demonstrate the accuracy of the polarization control, we have performed a detailed study summarized in Fig. 8. In this study, the input polarization state, ${\bf s}_{\rm in}$, was driven along a circular trajectory in one of the principal planes of the Poincaré sphere: $S_{3}=0$, $S_{2}=0$, or $S_{1}=0$. This was achieved by the free-space polarization generator depicted in the top panels (that is, (a), (d), and (g)) for each trajectory. The experimental data for the directional coupler’s outputs and the scattering intensity were collected after the polarization compensation procedure. We note that spin-locking and asymmetric dipolar emission effects produce comparable modulations of the directionality characterized by $P_{\Delta}$, see Figs. 8(c),(f). The higher noise in the ‘$-$’ channel (especially noticeable in Fig. 8(b)) was repeatable over numerous experimental attempts and independent of the detectors. The noise levels in the two channels were closer to each other for thicker nanofibers (with radii over 250 nm). Therefore, we attribute this effect to higher sensitivity of thinner nanofibers to bends due to vibrations or sagging, and, perhaps, to unknown deviations of the generated trajectory from the target one.

Our results contradict the general belief that short lengths of straight tapered fibers do not change the polarization by much and, even if they do, the shifts of the input state, ${\bf s}_{\rm in}$, by the down- and up-tapers are equal, so that the state at the waist, ${\bf s}_{\rm w}$, lies in the center between ${\bf s}_{\rm in}$ and ${\bf s}_{\rm out}$. According to our findings, presented in Fig. 1(b) and Fig. 7(b), the transformation matrices ${\rm M}_{-}$ and ${\rm M}_{+}$ lead to oppositely-directed, non-equal shifts of significant magnitudes. Therefore, it is clear that experiments with high levels of precision (like those involving quantum emitters) do require near-field polarization control, which can now be achieved using the reported method.

VI VI. Conclusion

We demonstrated the first method for the complete control of polarization of light in a single-mode optical nanofiber waveguide, using directional coupling between two such nanofibers. Although based on complex physical phenomena (the spin-momentum locking and the newly discovered asymmetric dipolar emission), our method is surprisingly simple and highly reliable. We believe that it will have significant impact on the vast range of experimental systems based on optical nanofibers and evanescently coupled elements, in general. The demonstrated directional coupler itself is a promising platform for developing integrated photonic circuits.

Acknowledgments

The authors would like to thank S. P. Mekhail for help with automation of the experiment, K. Karlsson for assistance with nanofiber fabrication, and F. Le Kien for helpful discussions. This study was partially supported by the Okinawa Institute of Science and Technology Graduate University. G. T. was supported by the Japan Society for the Promotion of Science (JSPS) as an International Research Fellow (Standard, ID No.P18367).

VII Appendix: polarization compensation requires non-orthogonal states

Our polarization compensation is based on sequential mapping of two input polarization states, $\bf A$ and $\bf B$, onto themselves at the waist of an optical nanofiber. As a result,

[TABLE]

where the unknown phase factors, $\delta_{A}$ and $\delta_{B}$, do not change the state, and the Jones matrix, $u=u_{\rm fiber}u_{\rm PC}$, describes the polarization transformation in the compensator ($u_{\rm PC}$) and the tapered fiber until the waist ($u_{\rm fiber}$). Since $u$ is unitary, the inner product of these states

[TABLE]

If these two states are not orthogonal, that is

[TABLE]

then Eq. 8 requires $\delta_{A}=\delta_{B}=\delta$. Under this condition, an arbitrary input state, $\bf C$, can be defined in the basis ($\bf A$, $\bf B$):

[TABLE]

where $a$ and $b$ are complex coefficients. Such a state $\bf C$ will be maintained in the polarization-compensated nanofiber.