Research Article | Open Access

Gerald T. Moore, "Model for a Torsional-Mode Ultrasonic Transducer for an Acousto-Optic In-Fiber Isolator", *Advances in OptoElectronics*, vol. 2010, Article ID 823157, 10 pages, 2010. https://doi.org/10.1155/2010/823157

# Model for a Torsional-Mode Ultrasonic Transducer for an Acousto-Optic In-Fiber Isolator

**Academic Editor:**Pierre Bourdon

#### Abstract

Torsional ultrasound modes can couple the optical polarization states in a birefringent fiber. Polarization coupling produced by interaction with a higher-order torsional mode slightly above its cutoff may provide a route to producing an in-fiber isolator suitable for use in narrow-band high-power fiber amplifiers. This paper describes a model of a transducer generating torsional modes in a cylindrical fiber. This model predicts that almost all of the power applied to the transducer is radiated into the desired mode. The paper also discusses effects produced by acoustic absorption and the dependence of the acoustic velocity on temperature.

#### 1. Introduction

By matching the optical polarization beat length in a birefringent silica optical fiber to the axial wavelength of a traveling torsional wave of angular frequency propagating in the fiber, it is possible to couple light from one polarization to the other [1, 2]. When light is coupled from the slow polarization to the fast polarization, it is down-shifted in frequency by if the light and sound are copropagating, but up-shifted if the light and sound are counter-propagating. This nonreciprocal frequency shift can be used to make an in-fiber acousto-optic (AO) isolator. This requires placing two torsional transducers on the fiber separated by , where is the group velocity of light in the fast polarization. These transducers propagate sound in the same direction. One watt of acoustic power from each transducer is sufficient to couple 50% of the light from one polarization to the other over a few centimeters [2]. The polymer jacket is removed from the fiber in the interaction regions to prevent acoustic damping. The relative acoustic phase of the two transducers is adjusted such that in the forward direction all of the light at the wavelength of interest returns to the slow polarization, whereas in the backward direction all of the light at this wavelength goes into the fast polarization. Polarizers at both ends, such as 45-degree tilted fiber Bragg gratings [3], remove light in the fast polarization to make an isolator. To date an isolator based on torsional acoustic waves has not been made, but 100% polarization switching has been demonstrated using the lowest-order () torsional mode [1]. However, an analogous isolator was demonstrated using the lowest-order flexural mode at āMHz [4]. In this case coupling was between the two transverse modes of a two-mode fiber. Although a 22ādB extinction ratio was reported, the large *D*ā=ā11ām spacing between the transducers makes this approach unattractive for high-power operation. The key to decreasing this spacing is to increase , while using an acoustic mode for which phase matching is possible at high frequency. Raising the frequency to about 50āMHz reduces the spacing between transducers to about 1ām. Except for the short regions following the transducers where acoustic coupling occurs, the fiber between the transducers can be coiled and jacketed with polymer. Figure 1 shows the layout of an AO isolator at four different length scales.

The phase-matching acceptance for polarization switching, which occurs over a few centimeters, is much wider than the transmission features produced by the transducer spacing and the linear polarizers. The transmission in the forward direction as a function of wavelength is a comb with periodicity , while the backward transmission is an out-of-phase comb. This is illustrated in Figure 2. The position of these combs depends on the relative acoustic phase of the two transducers. Hwang et al. [4] found that it was necessary to use a feedback circuit to adjust this phase to compensate for shifting of the combs produced by vibrations or temperature changes. The width of the comb maxima and minima is sufficient to prevent backward propagation of light produced by stimulated Brillouin scattering in narrow-band Yb-doped fiber amplifiers. The isolator can be used for multiple wavelengths commensurate with the comb period, such asthose thatmight be produced by spectral beam combination. However, it cannot protect against inadvertent lasing at other wavelengths within the gain bandwidth of Yb. This type of isolator can be tuned for use with other types of fiber amplifier besides Yb, such as Er or Tm.

A transducer spacing of 1ām imposes a power limitation on operation of an AO isolator, since undesirable nonlinear effects can build up over this distance. For example, we estimate that the nonlinear refractive index of fused silica will limit isolator operation to about 200āW in a 10ām core fiber and about 1ākW in a 25ām core fiber. By contrast, present fiber-coupled isolators are limited to about 50āW. Bulk isolators can withstand higher power but distort the beam quality at powers above about 100āW.

The frequency for phase-matching of the lowest-order torsional mode is too low for use as a high-power isolator, since becomes very large and the comb spacing very narrow. However, a transducer producing 100% polarization coupling with this mode can be used as a tunable notch filter [1], when placed between crossed polarizers. This can filter out undesired wavelengths, including wavelengths within the gain bandwidth of the amplifying medium.

#### 2. Matching of Transducer Modes and Free-Oscillation Modes

In the analysis below we consider the fiber to be a homogeneous elastic cylindrical glass rod, neglecting perturbations which might arise because of different elastic properties of the core or the stress rods. Torsional waves in a cylindrical rod are characterized by a displacement which is entirely in the azimuthal direction, but independent of the azimuthal coordinate . If the cylinder radius is , we can introduce a dimensionless frequency , where is the transverse sound velocity. This velocity is variously reported by Engan to be 3750ām/s [2] or 3764ām/s [5] in fused silica. Vacher et al. [6] found that at 5āMHz and 16āGHz are the same to within 0.1% at room temperature,suggesting that dispersion is small. However, was found to increase with temperature at 0.3ām/s kelvin. It is convenient to express and in units of . Then the torsional waves are of the form or , where .

The torsional modes of a free elastic cylinder are a subset of all the possible vibrational modes [7]. In general the displacement has an azimuthal dependence or . The modes with can be further subdivided into torsional and axial-radial. The modes with or higher are called flexural. The dispersion relations for the modes, except for the torsional modes, depend on the Poisson ratio for the material. Figure 3 shows the dispersion relations for (red) and (green) for the Poisson ratio 0.17 of fused silica. The lowest and highest red curves shown are the two lowest torsional modes. The other red curves are axial-radial. The lowest torsional, radial-axial, and flexural modes are the only ones with no cutoff. For torsional oscillations the two nonzero components of strain (with proportional components of stress) are and [8]. Our model for the transducer is a section of fiber between and where at is a single-frequency oscillation independent of . The model does not specify how such oscillation is produced. However, at the end of the paper we cite some methods that have been used to excite torsional vibrations in fibers and rods. at the surface of the fiber in the transducer, whereas at the surface of the free fiber. The displacement in the transducer is of the form where is the 'th zero of , , and is positive real for propagating modes or positive imaginary for cutoff modes. and are the modal amplitudes. We could multiply the first term above by a constant, but we choose to normalize in this way for now. Outside the transducer the fiber is uncontrained at the surface; so should vanish at . Since , we choose , where is the 'th zero of , and write the displacement for in the form where and is positive real for propagating modes or positive imaginary for cutoff modes. For positive the propagating modes with modal amplitudes carry power only in the positive direction. The mode with a cutoff at we call the mode. Since , the cutoff frequency for a fiber of diameter ām is āMHz. By operating just above the cutoff for the mode, we can match the axial wavelength to the optical polarization beat length (typically about 3āmm). The phase velocity approaches infinity at cutoff, while the sound group velocity approaches zero. The mode, corresponding to the term, has no cutoff, propagates at speed without dispersion, and can only be phase matched at much lower frequency. Since is greater than , a propagating mode inside the transducer already exists when passes through the cutoff.

At we write the displacement as Here are the modal amplitudes for sound propagating in the direction. The last two terms with amplitudes or are inserted to describe reflections of one of the modes above cutoff back into the transducer. For example, if the mode is above cutoff, we take to be nonzero and . The case of nonzero is not of much practical interest but is included for completeness. When the coefficients are zero, equal acoustic power is radiated from the transducer in both directions. The backward power is undesirable. It can be damped by leaving the jacket on the fiber at . However, more efficient operation might be possible by reflecting the power. For a mode near cutoff, reflection can be produced by raising the fiber temperature behind the transducer. This increases , which puts the mode below cutoff in this region. If the reflection is total, then , but the effects of the reflection depend on the phase of . This phase depends on the location of the thermal gradient producing the reflection and cycles through one period when this location shifts by half the longitudinal sound wavelength in the unheated fiber. Under phase-matched conditions this is also half the optical polarization beat length . Reflection should be produced close to the transducer in order to minimize AO coupling by light going in the direction.

At and both and should be continuous. This leads to the following set of four equations: Here we have introduced Note that in the absence of reflection (, ) we can take , , and , so that emission from the transducer is symmetrical.

The torsional modes outside the transducer are orthogonal, as can be seen from the following identities: Multiplying (4)ā(7) by either or , integrating, and using the above identities, we obtain We can eliminate , , , and from these equations to obtain a set of equations to be obeyed by and another set of equations to be obeyed by . In fact, if we define and , the equations derived from (12)ā(15) can be treated on the same footing as those derived from (16)ā(19). We obtain If one first specifies a value of (or ), these equations constitute a set of linear inhomogeneous equations for the amplitudes and . In order to solve these equations we choose an integer (typically 200) and truncate by letting run from 1 to and run from 0 to . Then we obtain and by numerical matrix inversion. The coefficients , , , and needed for the modal expansions of outside the transducer are then obtained from (12), (14), (16), and (18).

If, for example, one is interested in the situation where the mode is totally reflected at , we repeat the calculation for different values of in order to home in on the value of for which . The result depends on the phase of , which in turn depends on how and where the reflection occurs.

To check the convergence of our numerical procedure, we can plot the real and imaginary parts of the left and right sides of (4)ā(7) as a function of to see if they match. Equations (4) and (6) represent the displacements and , while (5) and (7) are proportional to the strain . We can also calculate from (4) and (6) to obtain expressions proportional to the strain . The real parts correspond to times when the transducer amplitude (the displacement at ) is maximal, while the imaginary parts correspond to times when the transducer amplitude is zero. In making these plots the number of terms we retain in the sums (typically 140) is less than , since the final terms can be corrupted by the matrix truncation.

We find that the matching of the external and internal displacements and strains is good. The differences appear as low-amplitude, high-frequency oscillations. The differences are most apparent in , which is zero at in the transducer but appears to be discontinuous as a function of at and when . The displacements and strains are insensitive to the choice of if is not too small.

#### 3. Energy Considerations

Since our model neglects sound absorption in the fiber, the power radiated in the modes which are above cutoff should equal the power applied to the transducer. Modes below cutoff are exponentially attenuated away from the transducer and do not propagate power. Let be the amplitude of the transducer motion at . Then the modal coefficients calculated in the previous section should be multiplied by to determine the physical displacement amplitudes. By comparison with the power expressions given in [2], we see that the power propagating in the mode at is , where and ākg/m^{2} is the density of fused silica. If, for example, nm, then āW. The power in higher-order modes which are above cutoff is . Analogous expressions apply to the power propagating at .

Division by is not possible when for some . In this case there is no steady state in the absence of damping. When , there is one propagating mode inside the transducer. We call this the mode. This mode can radiate only to the mode outside the transducer, and resonances occur as a function of . Internal values of are typically large compared to at the surface, and the power within the transducer can be much larger than the power driving the transducer. When exceeds , the channel opens, sound vibrations are no longer trapped in the transducer, the power is small, and the generated power is almost independent of . In general the power propagating in the forward and backward direction is given for modes above cutoff by To calculate the time-averaged power driving the transducer we use the stress evaluated at the surface of the fiber. The time-averaged power driving the transducer over the surface area is obtained by multiplying this stress by the surface velocity and averaging over time, Integrating over the surface of the transducer and using (8) and (10) yields It is often more meaningful to express powers relative to than in terms of .

#### 4. Numerical Results

Let us begin by considering a transducer with and , slightly above the cutoff. For a fiber with a diameter of ām this corresponds to a frequency āMHz and an axial wavelength āmm, on the order of the polarization beat length in polarization-maintaining optical fibers. One watt of power in this mode corresponds to an amplitude at of 85.7ānm. At this frequency the wavelength m is much too small for phase matching. We wish to compare the situation where the sound is emitted equally in both directions to the case where the mode is perfectly reflected at with phase or . is held constant in Figures 4 and 5, but depends on whether there is reflection. The red curves are at with reflection, the green curves are at with reflection, and the blue curves are at either end with no reflection.

**(a)**

**(b)**

**(c)**

**(d)**

**(e)**

**(f)**

**(a)**

**(b)**

**(c)**

**(d)**

**(e)**

**(f)**

In the case , with reflection, but with no reflection. Thus, reflection acts to reduce the power needed to drive the transducer to a given amplitude but does not greatly affect the way the transducer vibrates. The modal efficiencies with reflection are %, %, and %. % propagates in each direction between the point of reflection and . Within the transducer % and %. The amplitude at of the mode is .

In the case , ; so it becomes much harder to drive the transducer to a given amplitude . The modal efficiencies are %, %, and %. Thus, the transducer becomes a poor emitter of ultrasound, although a large power % propagates in each direction in the region between the point of reflection and the left end of the transducer. Within the transducer % and %. The transducer motion is qualitatively quite different because of the reflection.

In Figure 6 we plot the efficiency as a function of . We see that the efficiency is high over a broad range. On the other hand, without reflection 49.73% of the applied power is emitted into the mode in each direction, and the undesirable backward sound must be damped to prevent interaction with light in the fiber core.

The transducer simulations described below are for no reflections at . Above the cutoff the applied power and the radiated power are only weakly dependent on . Figure 7 shows the efficiency for each direction as a function of at . The and internal powers are much smaller than the power. The situation is different below the cutoff, where acoustic energy can leave the transducer only in the channel. This is illustrated in Figure 8 for , such that . While the efficiency for generating the mode in each direction remains at (red), goes to zero at resonances when is a multiple of (blue). Consequently the ratio becomes large near these resonances (green). We expect that damping effects not included in our model will act to suppress these resonances, but it may be best to avoid them by a suitable choice of .

In order to increase the frequency , so as to shorten the distance between the two transducers in an isolator, or to use a larger-diameter fiber, it is of interest to consider increasing above the cutoff for higher-order modes. Figure 9 shows the efficiency as a function of at , slightly above the cutoff (red). This figure also shows the efficiency at , slightly above the cutoff (green). We see that, as desired, most of the acoustic power goes into the mode that is just above cutoff. Scaling to large will eventually be limited by the increased attenuation of ultrasound at very high frequencies.

At , just below the cutoff, there is no dominance of over . Figure 10 shows (red) and (green), as well as the internal resonances (blue) and (violet). The and efficiencies in each direction sum to .

#### 5. Acousto-Optical Coupling, Acoustic Attenuation, and Thermal Effects

According to Engan [2] the coupling of the optical polarization states by phase-matched torsional acoustic waves is sinusoidal. That is, one polarization amplitude increases as , while the other decreases as . Here is position (not in units of ) along the fiber. We call the coupling angle. The coupling constant for the mode, provided that mode is above cutoff, is where is the acoustic power injected at into the phase-matched mode. Coupling of 50% of the light from one polarization to the other occurs over a distance . For 1āW of power in a fiber with a āmm polarization beat length and a ām diameter, the coupling length for the mode is ācm and the phase-matching frequency is 49.06āMHz. For the same power and beat length, but a ām diameter, the coupling length for the mode is ācm and the phase-matching frequency is 70.66āMHz.

When one takes damping of the sound waves into account, the power decreases exponentially after the sound leaves the transducer at . This means that has an imaginary part even above cutoff. The coupling angle at position now becomes . This means that a coupling angle of is only possible if , where the absorption length is defined as . The acoustic power decays as . When there is damping the distance over which sufficient coupling occurs is greater than .

We assume that the damping of the mode is the same as that found for transverse sound waves in bulk fused silica. Room-temperature measurements by Krischer [9] in the 200 to 1000āMHz range found the power attenuation to be , where . This agrees well with the value given by Kulābitskaya and Shutilov [10] but is smaller than the value reported by Fraser et al. [11]. Measurements by Krause [12] at 590āMHz showed a decrease in attenuation with increasing temperature with a minimum at about 375āC. For the present discussion we assume that Krischer's result can be extrapolated to lower frequencies. Dividing by and neglecting dispersion in the speed of sound, we find that m or , where .

For the mode is the total wave vector, and the transverse wave vector is zero. For higher-order modes we take , since the transverse wave vector is . Note that damping smears out the cutoff, and that has both real and imaginary parts on either side of the cutoff. Suppose that the beat length is āmm. For the example above of m and āMHz, the absorption length for the mode is ācm. The minimum power required at to achieve 50% optical coupling is āW. The mode in this fiber at 80.39āMHz has ācm and requires at least āW. For the example m and āMHz, the absorption length for the mode is ācm and at least 2.87āW in this mode is required. Absorbed acoustic power can produce a temperature gradient along the fiber. This can cause a chirp in , adversely affecting phase matching with the optical field. On the other hand, the phase-matching acceptance increases when the AO coupling length decreases. Heating can also be caused by optical power in the cladding. Cladding light can be removed before the isolator by embedding a section of fiber in high-index material. Air flow past the fiber can also reduce temperature gradients.

Even in the absence of temperature gradients and acoustic damping, the temperature dependence of [6] affects the cutoff frequencies and the phase-matching conditions. Figure 11 shows the axial sound wavelength as a function of temperature for fibers with diameters to m. The frequency āMHz is chosen to give an axial wavelength of 3āmm at 20āC in a m fiber. To the right of the cutoff resonances the ordinate is the distance over which the power decreases by . If the fiber diameter were to be slightly different at the locations of the two transducers in an isolator, phase matching for both transducers at the same frequency could be maintained by having the transducers at different temperatures. Backward acoustic power produced by a transducer can be reflected by heating the fiber behind the transducer over a sufficient length to prevent tunneling through the region where the reflected mode is below cutoff. The phase of the reflected light depends on how and where this heating is done.

#### 6. Discussion

Using higher-order torsional acoustic modes near cutoff to couple optical polarization states in a birefringent fiber allows phase matching to the polarization beat length at high frequencies in the 50āMHz range. Two torsional-mode transducers producing 50% polarization coupling and separated on the fiber by about 1ām can be used as an in-fiber optical isolator suitable for use with narrow-band fiber amplifiers of arbitrary wavelength. We have presented an analytical and numerical model of a torsional-mode transducer. This model indicates that the mode just above cutoff radiates most of the acoustic power applied to the transducer, irrespective of the transducer length. In the absence of acoustic reflection the power is radiated equally in both directions, and undesirable backward radiation must be absorbed. Reflecting the backward radiation towards the transducer with a suitable phase can enhance the efficiency in the forward direction to almost 100%.

Various types of transducers have been developed for exciting torsional vibrations in fibers or rods, but not at the high frequencies needed for an AO isolator. Transducers for exciting the mode in optical fibers have used a conical glass horn with the fiber mounted along its axis and shear-mode piezoelectric transducers attached to its base [1, 13ā15]. Other torsional transducers have been developed which use paired [16] or segmented [17, 18] piezoelectric elements. Torsional oscillations in metallic rods have been produced by electromagnetic-acoustic transduction [19]. Silicon-based micro-electromechanical systems (MEMSs) technology may provide a route to making higher-frequency torsional transducers. We are working with Sandia National Laboratories to explore this possibility.

#### Acknowledgments

The author would like to thank Chunte A. Lu for useful discussions. This research was supported in part by the High-Energy Laser Joint Technology Office.

#### References

- K. J. Lee, H. C. Park, H. S. Park, and B. Y. Kim, āHighly efficient all-fiber tunable polarization filter using torsional acoustic wave,ā
*Optics Express*, vol. 15, no. 19, pp. 12362ā12367, 2007. View at: Publisher Site | Google Scholar - H. E. Engan, āAnalysis of polarization-mode coupling by acoustic torsional waves in optical fibers,ā
*Journal of the Optical Society of America A*, vol. 13, no. 1, pp. 112ā118, 1996. View at: Google Scholar - K. Zhou, G. Simpson, X. Chen, L. Zhang, and I. Bennion, āHigh extinction ratio in-fiber polarizers based on ${45}^{\u0101\x88\x98}$ tilted fiber Bragg gratings,ā
*Optics Letters*, vol. 30, no. 11, pp. 1285ā1287, 2005. View at: Google Scholar - I. K. Hwang, S. H. Yun, and B. Y. Kim, āAll-fiber-optic nonreciprocal modulator,ā
*Optics Letters*, vol. 22, no. 8, pp. 507ā509, 1997. View at: Google Scholar - H. E. Engan, B. Y. Kim, J. N. Blake, and H. J. Shaw, āPropagation and optical interaction of guided acoustic waves in two-mode optical fibers,ā
*Journal of Lightwave Technology*, vol. 6, no. 3, pp. 428ā436, 1988. View at: Publisher Site | Google Scholar - R. Vacher, J. Pelous, F. Plicque, and A. Zarembowitch, āUltrasonic and brillouin scattering study of the elastic properties of vitreous silica between 10 and 300āK,ā
*Journal of Non-Crystalline Solids*, vol. 45, no. 3, pp. 397ā410, 1981. View at: Google Scholar - R. N. Thurston, āElastic waves in rods and clad rods,ā
*Journal of the Acoustical Society of America*, vol. 64, no. 1, pp. 1ā37, 1978. View at: Google Scholar - A. I. Beltzer,
*Acoustics of Solids*, Springer, Berlin, Germany, 1988. - C. Krischer, āOptical measurements of ultrasonic attenuation and reflection losses in fused silica,ā
*Journal of the Acoustical Society of America*, vol. 48, pp. 1086ā1092, 1970. View at: Google Scholar - M. N. Kul'bitskaya and V. A. Shutilov, āUltrasonic investigation of glasses (review),ā
*Soviet PhysicsāAcoustics*, vol. 22, pp. 451ā461, 1976. View at: Google Scholar - D. B. Fraser, J. T. Krause, and A. H. Meitzler, āPhysical limitations on the performance of vitreous silica in high-frequency ultrasonic and acousto-optical devices,ā
*Applied Physics Letters*, vol. 11, no. 10, pp. 308ā310, 1967. View at: Publisher Site | Google Scholar - J. T. Krause, āGold-indium bond for measurement of ultrasonic properties in solids at high temperatures,ā
*Journal of Applied Physics*, vol. 39, no. 11, pp. 5334ā5335, 1968. View at: Publisher Site | Google Scholar - K. J. Lee, K. S. Hong, H. C. Park, and B. Y. Kim, āPolarization coupling in a highly birefringent photonic crystal fiber by torsional acoustic wave,ā
*Optics Express*, vol. 16, no. 7, pp. 4631ā4638, 2008. View at: Publisher Site | Google Scholar - M. Berwick, C. N. Pannell, P. ST. J. Russell, and D. A. Jackson, āDemonstration of birefringent optical fibre frequency shifter employing torsional acoustic waves,ā
*Electronics Letters*, vol. 27, no. 9, pp. 713ā715, 1991. View at: Google Scholar - M. Berwick and D. A. Jackson, āCoaxial optical-fiber frequency shifter,ā
*Optics Letters*, vol. 17, pp. 270ā272, 1992. View at: Google Scholar - J. Friend, K. Nakamura, and S. Ueha, āA torsional transducer through in-plane shearing of paired planar piezoelectric elements,ā
*IEEE Transactions on Ultrasonics, Ferroelectrics, and Frequency Control*, vol. 51, no. 7, pp. 871ā878, 2004. View at: Google Scholar - N. Tsubouchi, āResonator for torsional vibration,ā US patent no. 3,774,057, November 1973. View at: Google Scholar
- J. O. Kim and O. S. Kwon, āVibration characteristics of piezoelectric torsional transducers,ā
*Journal of Sound and Vibration*, vol. 264, no. 2, pp. 453ā473, 2003. View at: Publisher Site | Google Scholar - W. Johnson, B. A. Auld, and G. A. Alers, āSpectroscopy of resonant torsional modes in cylindrical rods using electromagnetic-acoustic transduction,ā
*Journal of the Acoustical Society of America*, vol. 95, no. 3, pp. 1413ā1418, 1994. View at: Google Scholar

#### Copyright

Copyright © 2010 Gerald T. Moore. This is an open access article distributed under the Creative Commons Attribution License, which permits unrestricted use, distribution, and reproduction in any medium, provided the original work is properly cited.